Spin-polarized scanning tunneling microscopy with quantitative insights into magnetic probes

Soo-hyon Phark; Dirk Sander

doi:10.1186/s40580-017-0102-5

Review
Open Access
Published: 06 April 2017

Spin-polarized scanning tunneling microscopy with quantitative insights into magnetic probes

Soo-hyon Phark^1,2 &
Dirk Sander³

Nano Convergence volume 4, Article number: 8 (2017) Cite this article

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Abstract

Spin-polarized scanning tunneling microscopy and spectroscopy (spin-STM/S) have been successfully applied to magnetic characterizations of individual nanostructures. Spin-STM/S is often performed in magnetic fields of up to some Tesla, which may strongly influence the tip state. In spite of the pivotal role of the tip in spin-STM/S, the contribution of the tip to the differential conductance dI/dV signal in an external field has rarely been investigated in detail. In this review, an advanced analysis of spin-STM/S data measured on magnetic nanoislands, which relies on a quantitative magnetic characterization of tips, is discussed. Taking advantage of the uniaxial out-of-plane magnetic anisotropy of Co bilayer nanoisland on Cu(111), in-field spin-STM on this system has enabled a quantitative determination, and thereby, a categorization of the magnetic states of the tips. The resulting in-depth and conclusive analysis of magnetic characterization of the tip opens new venues for a clear-cut sub-nanometer scale spin ordering and spin-dependent electronic structure of the non-collinear magnetic state in bilayer high Fe nanoislands on Cu(111).

Background

Nanoscopic magnetic tunnel junction in STM

Spin-polarized scanning tunneling microscopy and spectroscopy (spin-STM/S) is a magnetic imaging technique with an ultimate lateral resolution on the atomic scale [1–4], which is suitable for probing magnetism in ferromagnetic nanostructures [5–7] and in antiferromagnets [8–10]. Figure 1a schematically describes electron tunneling in spin-STM. Electrons carry spin as well as charge, thus the electron tunneling is spin dependent [11–13]. When magnetically ordered materials are used for both tip and sample, the tunneling current depends on the magnetic order parameters of both tip and sample (here the local magnetization, M _T and M _S, respectively). In addition, spin-STM under an external field μ₀ H allows to control the orientations of M _T and M _S. This is the basis to use spin-STM, undoubtedly, to perform a ‘magnetic tunneling junction’ (MTJ) experiment on the single atom level.

A spatially resolved measurement of the differential conductance dI/dV of the tunnel current provides a spatial map of electronic information relevant to the local magnetic order. Figure 1b, c are schematics describing the spin-dependent tunneling in (b) parallel (P) and (c) antiparallel (AP) configurations between M _T and M _S. The electronic density of states (DOS) of ferromagnets splits up into majority (n ^↑)- and minority (n ^↓)-spin DOSs due to exchange interaction between electrons [14], giving rise to the spin polarization P(E) at a given energy E.

$$P\left( E \right) = \frac{{n^{ \uparrow } (E) - n^{ \downarrow } (E)}}{{n^{ \uparrow } \left( E \right) + n^{ \downarrow } (E)}}$$

(1)

Assuming (a) identical DOSs for both sample and tip and (b) conservation of spin orientation during the tunneling process, the schematic implies that the tunneling current will depend on the magnetization configurations (P or AP), as depicted by the thickness of the curved black arrows. It is plausible that one can derive the contribution arising from the spin-polarization P(E) explicitly in the mathematical formula of the tunneling phenomena. Thereby, it is instructive to write the tunneling current at the tip position R _T as

$$I\left( {\varvec{R}_{T} ;V;\theta } \right) = I_{0} \left( {\varvec{R}_{T} ;V} \right) + I_{P} \left( {\varvec{R}_{T} ;V;\theta } \right),$$

(2)

where I ₀ and I _P denote the non-spin-polarized and spin-polarized currents, respectively, and $\theta \;( \equiv \theta_{\text{T}} {-}\theta_{\text{S}} )$ is the angle between M _T and M _S, as depicted in Fig. 1a.

Spin-dependent differential conductance dI/dV in spin-STS

Wortmann et al. developed a theoretical description of the tunneling current in spin-STM [15]. According to Bardeen’s approach [16], the tunneling current is written as

$$I\left( {\varvec{R}_{{\mathbf{T}}} , V} \right) = \frac{2\pi e}{\hbar }\mathop \sum \limits_{\mu ,v} \left[ {f\left( {\upvarepsilon_{\mu }^{S} - \varepsilon_{F} } \right) - f\left( {\upvarepsilon_{\mu }^{T} - \varepsilon_{F} } \right)} \right] \times \delta \left( {\upvarepsilon_{\nu }^{T} -\upvarepsilon_{\mu }^{S} - eV} \right)\left| {M_{\nu ,\mu } \left( {\varvec{R}_{{\mathbf{T}}} } \right)} \right|^{2} ,$$

(3)

where R _T, V, $f(\upvarepsilon)$, $\upvarepsilon_{\mu /v}^{{{\text{T}}/{\text{S}}}}$, and $\upvarepsilon_{\text{F}}$ are the tip position, the bias voltage, the Fermi function, the tip/sample energy states, and the Fermi energy, respectively. To calculate the matrix elements $M_{\nu ,\mu } \left( {\varvec{R}_{\text{T}} } \right) = \langle{\varPsi }_{\nu }^{\text{T}} \left| {U_{\text{T}} } \right.\left| {{\varPsi }_{\mu }^{\text{S}} \rangle,} \right.$ the authors introduced the two component spinors for the tip and sample wave functions Ψ ^T_ν and Ψ ^S_μ , respectively,

$$\varPsi_{\nu }^{T} = \left( {\begin{array}{*{20}c} {\psi_{\nu \uparrow }^{T} } \\ 0 \\ \end{array} } \right)\quad {\text{or}} \quad \varPsi_{\nu }^{T} = \left( {\begin{array}{*{20}c} 0 \\ {\psi_{\nu \downarrow }^{T} } \\ \end{array} } \right) ,\quad \varPsi_{\mu }^{S} = \left( {\begin{array}{*{20}c} {\psi_{\mu \uparrow }^{S} } \\ {\psi_{\mu \downarrow }^{S} } \\ \end{array} } \right)$$

(4)

The authors also introduced the ‘magnetization density of states’ m(E) to account for the decisive role of the relative orientation between M _T and M _S in the tunneling of spin-STM,

$$\varvec{m}\left( E \right) = \left( {n^{ \uparrow } - n^{ \downarrow } } \right)\hat{\varvec{e}}_{\text{M}} = nP\left( E \right)\hat{\varvec{e}}_{\text{M}} ,$$

(5)

where n ^↑ (n ^↓) is the spin-up (-down) DOS at energy E, and $\hat{\varvec{e}}_{\text{M}}$ is the unit vector of the magnetization. Assuming spin-conserved tunneling and constant tip DOS [17], substitution of the spinors (Eq. 5) leads to

$$\begin{aligned} I\left( {\varvec{R}_{\text{T}} , V,\theta } \right) = \frac{{8\pi^{3} C^{2} \hbar^{3} e}}{{\kappa^{2} m^{2} }}\mathop \int \nolimits {d\varepsilon } \left[ {f\left( {\upvarepsilon -\upvarepsilon_{F} } \right) - f\left( {\upvarepsilon + eV -\upvarepsilon_{F} } \right)} \right]\mathop \sum \limits_{\mu } \delta \left( {\upvarepsilon_{F} -\upvarepsilon} \right) \hfill \\ \;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\; \times \left[ {n_{\text{T}}^{ \uparrow } \left| {\psi_{\mu \uparrow }^{\text{S}} \left( {\varvec{R}_{\text{T}} } \right)} \right|^{2} + n_{\text{T}}^{ \downarrow } \left| {\psi_{\mu \downarrow }^{\text{S}} \left( {\varvec{R}_{\text{T}} } \right)} \right|^{2} } \right], \hfill \\ \end{aligned}$$

(6)

where $\theta \left( {\varvec{R}_{\text{T}} , V} \right)$ denotes the angle between M _T and M _S.

The differential conductance dI/dV measurement in the spin-STS provides a quantity which is directly correlated to the projection of the spin-DOS of the sample onto that of the tip at the tip position R _T. Recalling the description of Eq. 2, and using a set of algebraic processes [15], the Eq. 6 gives

$$\frac{{\text{d}I}}{{\text{d}V}}\left( {\varvec{R}_{\text{T}} , V} \right) \propto n_{\text{T}} n_{\text{S}} \left( {\varvec{R}_{\text{T}} ,\upvarepsilon_{\text{F}} + eV} \right) + \varvec{m}_{\text{T}} \cdot \varvec{m}_{\text{S}} \left( {\varvec{R}_{\text{T}} ,\upvarepsilon_{\text{F}} + eV} \right),$$

(7)

which exhibits a non-magnetic (1st term; dI/dV|₀) and magnetic (2nd term; dI/dV|_mag) term explicitly. Note, that the second (magnetic) term results in $n_{\text{T}} n_{\text{S}} P_{\text{T}} P_{\text{S}} \hat{\varvec{e}}_{\text{M}}^{\text{T}} \cdot \hat{\varvec{e}}_{\text{M}}^{\text{S}}$, which is proportional to the projection of M _S to M _T at the tip position.

Experimental approach

The experiments were performed in situ in an ultra-high vacuum (UHV) chamber (base pressure <1 × 10⁻¹¹ mbar) equipped with a liquid He cooled scanning tunneling microscope operating at 10–30 K and a superconducting magnet for field of up to 7 T normal to the sample surface [4, 18].

Co and Fe nanostructures on Cu(111)

Here we focus on biatomic-layer-high (BLH) Co, Fe, and Fe-decorated Co (Fe|Co) islands on Cu(111) [7, 18–20]. Figure 2a schematically illustrates the sample preparation procedure. It results in 3 types of BLH islands schematically depicted in Fig. 2b: First, a sub-monolayer (ML)-equivalent Co deposition at room temperature (RT) forms Co islands as shown in Fig. 2c. Constant current STM (CC-STM) image of the sample surface formed by 0.5 ML-equivalent Co reveals an island height of ~4 Å, indicative of BLH Co. The islands have a lateral dimension ranging from 5 to 30 nm. Second, the sequential deposition of first sub-MLs of Co (0.24 ML) and then Fe (0.28 ML) at RT formed two types of islands (Fig. 2d): (1) pure BLH Fe island; (2) BLH Fe|Co island, where Co forms the core and Fe surrounds the Co perimeter. We performed spin-polarized STM and STS on individual islands for all three types of islands.

Spectroscopic identification of element-specific electronic structures of nanoislands

We discriminate different surface regions (Co, Fe, and Cu) in the STM images (Fig. 2c and d) by differences in apparent heights. Those regions are also identified spectroscopically by local STS measurements. Figure 2e shows five STS spectra measured at the positions indicated by the numbers 1–5 in Fig. 2d, where the same color code is used. Spectra 1 and 3 exhibit the onsets of the surface states of Cu(111) [21] and the 3d _z2-minority state of Co [22] at the respective characteristic bias voltages V _b = −0.4 and −0.3 V. STS identifies two electronically different Fe regions. BLH Fe on Cu(111) has two structurally and electronically different phases [23, 24]. Spectrum 4 shows a dominant peak at −0.39 V and a small peak at −0.03 V. This is the signature of the electronic structure of BLH Fe in fcc-stacking [24]. Spectrum 5 shows a peak at −0.22 V, and it is almost indistinguishable from the spectrum measured at position 2 in the pure Fe island. These spectra indicate BLH Fe in bridge-site-stacking of topmost Fe atoms [23, 24].

Spin-polarized STM/S and dI/dV mapping

For non-magnetic STM/S measurements, we used electrochemically etched W tips. For spin-STM/S, we used either Fe-coated W tips [19] or Cr/Co-coated W tips [5, 7, 25]. Details of the sample and tip preparations are described in Refs. [7] and [19]. STS spectra were measured by employing a lock-in technique with a modulation V _b at a frequency v = 4 kHz and a root-mean-square amplitude of 20 mV to detect the tunnel current I(V) and the differential conductance dI/dV simultaneously. In order to obtain the switching field H _sw of an individual island, the differential conductance magnetic hysteresis loop dI/dV(H) was measured at the center of the Co core of the island with an external field μ₀ H sweep up to 3 T. The H _sw of the island was extracted from the sharp drop of the signal in the dI/dV(H) hysteresis loop. For a simultaneous measurement of CC-STM and spin-polarized dI/dV images, we utilized the spectroscopic mapping technique under an external magnetic field. The field value and the field history is chosen such that at the same field value AP and P magnetization configurations are realized. After taking STS spectrum at each location of a scan for varying the bias voltage, we extract the dI/dV signal for every pixel at a given energy. Thus, we obtain energy-resolved dI/dV maps of an island for both AP and P magnetization configurations. To obtain a spatial resolution on the atomic scale (<2 Å), we chose a pixel number larger than 150 × 150 for a 25 × 25 nm² image size. This corresponds to a measurement time of 12 h order for a spectroscopic map.

Field dependence of differential conductance in spin-stm

Spin-STM of Co nanoislands on Cu(111)

Figure 3a shows a STM image of typical BLH Fe|Co islands on Cu(111). The Co core regions of the islands are enclosed by dotted lines and labeled by ‘1’ and ‘2’, [19]. The crosses mark the location of the dI/dV measurements. Spin-STM measurements were carried out using Fe-coated W tips in an external magnetic field μ₀ H, as schematically illustrated in Fig. 3b, at a sample temperature of 10 K.

Figure 3c shows the STS spectra measured at the center of Co core 1, as marked by the red cross in Fig. 3a, under varying μ₀ H along the surface normal. The STS spectra show at all field values the sharp 3d _z2-related electronic state of Co near V _b = −0.3 V [22], as indicated by the black vertical arrow. Shape and amplitude of the spectra change with magnetic field. We identify a bias voltage V _b = −0.87 V, which gives a clear field-dependent change of the dI/dV signal. Figure 3d shows the dI/dV hysteresis loop extracted from the dI/dV values at V _b = −0.87 V. The hysteresis loop consists of butterfly-shaped curves, which are symmetric about the vertical axis [25, 26]. The sudden drop of the signal at ±1.6 T indicates the switching of the magnetization direction of the Co core [6]. A gradual change of the dI/dV signal is observed in the field range below the switching field H _sw, implying that the out-of-plane component of the tip magnetization varies with the external field [25].

Probing methods of spin-STM

Spin-polarized tips

Spin-polarized tips are an important ingredient for spin-STM. Several experimental schemes for obtaining spin-polarized tips have been proposed, which were already realized in planar tunnel junctions: (1) magnetic materials [13, 27–29], (2) optically pumped GaAs [30], and (3) superconducting materials in magnetic fields [11, 12, 31, 32] have been used in spin-dependent transport measurements.

Modulation of tip magnetization method

A mode of spin-STM operation, where a tiny coil is used for periodically switching the tip magnetization back and forth, was introduced by Wulfhekel et al. [33]. If the modulation frequency exceeds the cutoff frequency of the feedback loop, the measured signal becomes proportional to the local magnetization of the sample. This method can effectively separate topographic and electronic from magnetic contrast effects for a given sample bias. However, this approach appears to be highly demanding and time consuming compared to the simple measure of the STM signal using a spin-polarized tip. Another limitation of this method is that ferromagnetic tips have to be used, which is not free from the effect of its stray field on the measured magnetic contrast. Despite, recently near-atomic resolution has been achieved on a reconstructed Mn film epitaxially grown on a Fe(001) substrate using the modulated tip magnetization mode [34].

Tunneling anisotropic magnetoresistance (TAMR) effect

There are some reports which claim to observe spin-contrast for tips with no spin-polarization [35–37]. In principle the tunnel current—even from a non-spin-polarized tip—depends on the magnetization direction of the sample and a magnetic contrast is feasible. This tunneling anisotropic magnetoresistance (TAMR) has been reported for W-tips. The significance of TAMR for spin-STM is difficult to judge, as material exchange form the magnetic sample onto the tip cannot be excluded exclusively.

Tips made of magnetic materials

All results presented in this review were obtained using tips of magnetic materials. Common ways of preparing tips of magnetic materials are either coating W-tips with magnetic materials or direct electrochemical etching of bulk magnetic materials [38, 39]. Using a bulk antiferromagnetic material such as Cr [25, 26] or MnNi diminishes the magnetic stray field emanating from the tip [40–43].

W tips coated by magnetic materials

A few sequential steps are applied to obtain Fe [19, 20], Cr [25], Cr/Co [5, 7, 25] -coated W tips: (1) ex situ preparation of W tips through electrochemical etching in 1.5 M NaOH solution. (2) flash heating of the etched W tip at a temperature above 2200 °C under UHV conditions to remove contaminants and W-oxides, and to partially crystallize the tip apex. (3) deposition of magnetic materials, such as Fe (40 AL-equivalent), Cr (20–100 AL-equivalent), or Co (40 AL-equivalent) followed by Cr (40 AL-equivalent) onto W tip apices for Fe-W, Cr-W, or Cr/Co-W tips, respectively. This deposition is followed by post-annealing at a mild temperature around 400 °C to recrystallize each magnetic coating for a stable structural phase at the tip apex. (4) in situ microscopic preparation by application of voltage pulses between tip and sample with a duration of typically a few ms to shape the tip apex. Just after each voltage pulse, the tip was tested by STS measurement on a surface with well-known spectroscopic features, such as the surface states of Cu(111) and bilayer Co island. The proper dI/dV signal indicates that the tip is usable in spin-STM measurements.

Cr-bulk tips

The tip was made of polycrystalline Cr rods with a nearly square cross section of 0.7 × 0.7 mm² obtained by cutting a 99.99% Cr foil (from Super Conductor Materials). The Cr rod was electrochemically etched in 1.5 M NaOH solution, following the procedure reported in Ref. [38] and then it was directly transferred into the STM. The only in situ preparation step was the application of voltage pulses on the Cu(111) surface to shape the apex [26].

Characterization of tips by field emission microscopy (FEM)

In the field emission microscopy (FEM), the electrons are extracted from the metal tip to the vacuum [44], thus, their spin polarization is proportional to that of the surface at the metal tip. Nagai et al. investigated the atomic structures and spin polarizations at the apex of Fe/W and Cr/W tips used in spin-STM by means of FEM and field ion microscopy (FIM) [45]. FIM has been used to investigate atomic structures at the apex of metal tips [46]. Thus, FEM combined with FIM can provide information of spin polarization of a tip correlated to its atomic structure. The FIM of the Fe/W tip showed that the deposited Fe layers form a single crystalline structure over the apex, except for the first few layers. The spin polarization at the surface is as high as 41.2%, which is attributed to the single crystalline structure of Fe. On the other hand, a FIM image of the Cr/W tip showed that the Cr layer was not well-ordered crystalline, although some hints of crystalline order were observed because of the Cr islands. Consequently, the spin polarization is as low as 10.3%. These results may allow one to prepare and characterize the structure of the magnetic tips and to quantify their spin polarization for use in spin-STM.

Magnetic responses of tips to the external field

Figure 4a–c show magnetic hysteresis loops of the dI/dV signal measured at the center of bilayer Co islands on Cu(111) using (a and b) Cr-W and (c) Cr/Co-W tips [25]. A first inspection of the data reveals a striking unexpected result that the same macroscopic preparation procedure of tips gives rise to vastly different hysteresis curves (compare Fig. 4a, b). To appreciate the shape of the hysteresis curves in Fig. 4a–c, it is important to realize that the field-driven change of the dI/dV signal is ascribed to a corresponding change of the relative orientation between the M _T and M _S [1].

The observed hysteresis curves are either (a) asymmetric or (b and c) symmetric about the vertical dI/dV axis. Figure 4d, e are schematic illustrations of the local magnetization configurations and of the magnetic response of a bilayer Co island to the external field, respectively. Due to the uniaxial out-of-plane magnetic anisotropy, the Co island exhibits only a bistable single domain magnetization state. The Wortmann formula (Eq. 7) consequently points at the response of the tip to the applied field, as schematically illustrated in Fig. 4f–h, respectively. Accordingly, the shape of the curve in Fig. 4a is ascribed to a fixed magnetization direction of the tip apex, which does not change in response to the external field, as sketched in Fig. 4f. On the other hand, the symmetric hysteresis curves in Fig. 4b and c indicate that here the magnetization direction of the tip apex has changed in response to the external field. The magnetic response in Fig. 4g indicates a gradual increase with external field of the out-of-plane component of the tip magnetization M _T,⏊ along the field direction, starting from 0 at zero field, and reaching saturation before the BLH Co core switches. A non-hysteretic field dependence of dI/dV(H) results for H < H _sw. Figure 4h represents a ferromagnetic state of the tip, where a switching of tip and sample at different field magnitudes is observed. The results presented in Fig. 4 imply a complex magnetic behavior of the tips, which even varies under the same macroscopic preparation. This indicates that, in addition to the macroscopic preparation, also the in situ microscopic tip preparation by voltage pulses is a further decisive aspect which determines the magnetic contrast in spin-STM.

Note that only the tips characterized by curves in Fig. 4a, c give rise to a magnetic contrast for an out-of-plane magnetized sample at zero field. Tips represented by the curve in Fig. 4b require an out-of-plane field to provide magnetic contrast for out-of-plane magnetized samples. Therefore, the results of Fig. 4 indicate that the magnetic contrast in spin-STM changes differently for a change of magnetic configuration of the tip.

It has been tacitly assumed that a high signal of the dI/dV in spin-STM corresponds to a P configuration, while a low signal corresponds to an AP configuration [47–49]. However, the results presented in Fig. 4 show that only in connection with a field sweep, a reliable deduction of the magnetic configurations from the dI/dV signal is warranted. A closer inspection of Fig. 4 reveals that the value of the dI/dV and its variation upon a change of the magnetic configuration varies from curve to curve, and it also differs for the same macroscopic preparation. The considerable difference of the magnetically induced signal ΔdI/dV (refer Fig. 3d; ~0.6 nS for Fig. 4a, ~3 nS for Fig. 4b) also reflects that a specific magnetic behavior is not necessarily linked to a certain macroscopic tip preparation. All the observations in Fig. 4 indicate that neither the material at the tip apex, nor its thickness, nor its spectroscopic features are parameters which are sufficient to determine the magnetic properties of the tip, but only field-dependent measurements do so.

Magnetic characterization of tips in spin-stm

To understand the tip contribution to the a dI/dV(H) signal requires a plausible physical description of M _T. We introduced in Sect. 2.4 various types of magnetic response of M _T to the applied field. However, it is still not sufficient due to the following complications: (1) The non-hysteretic field response illustrated in Fig. 4g can be caused by either a field-driven continuous rotation of M _T, which is originally in-plane oriented at zero-field, or by a superparamagnetic (SPM) response of M _T. In both cases the out-of-plane component of the tip magnetization M _T,⏊ increases with field, and a non-hysteretic and saturated field dependence of dI/dV(H) results. (2) The tip can also have an out-of-plane magnetic anisotropy with a large magnetic moment and exhibits a ferromagnetic response to the applied field, as illustrated in Fig. 4h. This reasoning can be applied to all cases shown in Fig. 4. This implies that the sharp change in all three dI/dV(H) curves could alternatively stem from the switching of the bistable M _T along the applied field direction instead of that of M _Co. In this section, we introduce some experimental approaches of resolving the abovementioned open issue and, thus, advancing spin-STM to be a tool for the quantitative measurement of nanomagnetism in samples by specific control of the external field.

Ferromagnetic tip

Figure 5a is a CC-STM image of bilayer Co islands on Cu(111) [50, 51]. Spin-STM of the Co islands was performed with a Cr/Co-coated W tip, as schematically described in Fig. 5b. Differential conductance spectra were measured at the center of two Co islands, marked by the dashed circles (red and black) in Fig. 5a. A pronounced magnetic field dependence of the dI/dV signal is observed [5], in the dI/dV hysteresis loops. Note the sharp signal drop at μ₀ H = ±0.5 T is observed on both islands. The steep jumps at μ₀ H = ±1.3 and ±0.8 T differs for red and black island. The switching field H _sw of the magnetization reversal of the BLH Co islands on Cu(111) strongly depends on the size of the islands [6, 47]. On the other hand, the H _sw of the tip would be the same provided the dI/dV measurements are performed with the tip apex. Thus, the sharp signal drop at μ₀ H = ±0.5 T must be ascribed to the reversal of M _T, and the steep increase at μ₀ H = ±1.3 and ±0.8 T is ascribed to the reversal of the magnetization of the larger (black) and the smaller (red) Co islands, respectively. The minor hysteresis loop in Fig. 5d, obtained under a field sweep between −1.2 and +1.2 T, where M _S keeps its direction pointing down, corroborates the discussion on the response of M _T to the external field. Here, a ferromagnetic tip with a switching field of ±0.5 T is observed.

Superparamagnetic tips

Magnetism on a nanometer scale strongly depends on the measurement temperature due to the impact of thermal fluctuations. This is described by the so called ‘superparamagnetic criterion’ 25k _B T ≥ K _a V, where k _B T and K _a V represent the thermal energy and the magnetic anisotropy energy, respectively [52]. If the tip response shown in Fig. 4g is caused by the field-driven rotation of the M _T from in-plane to out-of-plane, the magnetic anisotropy energy should be large enough to maintain the given magnetic state against thermal fluctuations. On the other hand, the field dependence of the dI/dV signal will depend strongly on the measurement temperature in case of a tip in the superparamagnetic state.

To address this ambiguity and to elucidate the physical origin of the tip response shown in the butterfly-shaped dI/dV(H) in Fig. 4b, we measured dI/dV(H) hysteresis curves at different temperature, where M _Co retains a fixed orientation (here pointing down). Figure 6a, b present the field dependence of dI/dV data measured at the center of the Co cores of the islands 1 and 2 shown in Fig. 3, respectively. We used a Fe-W tip at three temperatures, 10 K (black), 20 K (red), and 30 K (green). Note that the slope of the dI/dV signal at 0 T gets smaller with increasing temperature. At a fixed orientation of M _Co, we ascribe the observed change of the dI/dV(H) signal to the response of the tip to both field and temperature. Each data set of the same color code shows a saturation with increasing field, but the saturation field increases with increasing temperature. This suggests a superparamagnetic response of the tip.

To support and quantify this assertion, we analyze the temperature dependences of the dI/dV signal in Fig. 6a and b within the framework of superparamagnetism [52] by fitting each set of dI/dV data to a Langevin function

$$\frac{dI}{dV}\left( H \right) = \left( {\frac{dI}{dV}} \right)_{\text{sat}} \left[ {\coth \frac{{m_{\text{tip}} \mu_{0} \left( {H - H_{\text{off}} } \right)}}{{k_{\text{B}} T}} - \frac{{k_{\text{B}} T}}{{m_{\text{tip}} \mu_{0} \left( {H - H_{\text{off}} } \right)}}} \right] - \left( {\frac{dI}{dV}} \right)_{\text{C}}.$$

(8)

We introduce the saturation of the differential conductance (dI/dV)_sat and the differential conductance offset (dI/dV)_C, which determines the average of the two dI/dV saturation values for the P and AP magnetization configurations. We also introduce the offset field H _off, to consider the shift of the curves by 60 mT to the positive field direction, which tentatively ascribed to the stray field induced by M _Co. The dI/dV data are normalized to a saturation value of ±1. The solid curves through the data points of Fig. 6a, b are fits using Eq. 8, resulting in a magnetic moment m _tip = 660 ± 30 μ_B for all measurements.

The convincing description of the experimental data by the Langevin approach is further corroborated by plotting all data points as a function of μ₀ H/T. The condensation of all data on a single curve, as shown in Fig. 6c, is the hallmark of a superparamagnetic response [52]. In a first approximation, we ascribe the extracted magnetic moment to a macrospin, where all individual spins at the tip apex respond in unison to the external field. Assuming a magnetic moment of 2.2–3 μ_B per single Fe atom in Fe nanoclusters [53] leads us to speculate that a nano-apex of approximately 220–300 Fe atoms determines the magnetic response of this tip.

We use the ‘superparamagnetic criterion’ [52], to estimate the upper limit for the magnetic anisotropy as K _a ≤ 0.07–0.1 meV/atom for 300–220 Fe atoms, respectively. Thus, even a considerably increased magnetic anisotropy per Fe atom of the nano-apex as compared to bulk Fe (~0.0035 meV/atom) [54] would still fulfill the superparamagnetic criterion. In spite of the convincing description of our data with a macrospin model, we cannot exclude a more complicated arrangement of the magnetic structure at the nano-apex, which could also result in the same magnetic moment of 660 μ_B. We analyzed seven Fe-coated W tips, which were prepared under the same conditions as described above. In all cases we found a very good description of the experimental data by a superparamagnetic response. The analysis revealed a magnetic moment between 100 and 2000 μ_B for the different tips. This finding suggests that the same macroscopic tip preparation by Fe deposition followed by annealing may lead to different nano-apices with 30–900 Fe atoms, and these microstructures at the tip apex determine the magnetic response of the tip.

Tips with a Stoner-Wohlfarth-like magnetization response

Figure 7a shows a CC-STM image of a BLH Co island in contact with a Fe bilayer rim (Fe|Co island) [18, 19] and a pure Fe island. We performed field-dependent dI/dV measurements at the center of the Co core, which is indicated by the black dashed curve of the island A. We used a Cr/Co-coated W tip under an external field sweep between −3 and +3 T [7]. Figure 7b shows the dI/dV hysteresis loop, extracted from the dI/dV values of the Co spectra. It clearly shows two distinctive groups of dI/dV values, corresponding to the AP (intermediate field values) and P (high field values) magnetization configurations [5]. The changes of the dI/dV signal at ±0.24 T and ±1.1 T indicate the magnetization reversals of the tip and of the Co core, respectively, as discussed in the Sect. 3.1. Interestingly, a close inspection of the curve after subtraction of the signal change due to sample and tip reversal reveals a monotonic change of the dI/dV signal, which saturates at ∼ ±1.5 T.

To identify the magnetic state of the tip, we obtained a dI/dV hysteresis loop with a field sweep between −1 and +1 T, as shown by red and blue squares in Fig. 7c. This field regime is smaller than the switching field of the Co core, thus leaving the M _Co unchanged. Therefore, the field dependence of the dI/dV signal in Fig. 7c reflects solely the response of M _T to the applied field. Besides the magnetization switching at ±0.24 T, we note a monotonic dI/dV signal increase (decrease) for the backward (forward) field sweep. Based on the constant M _Co oriented in the out-of-plane direction, the field-dependence of the dI/dV signals in Fig. 7c implies a gradual increase of the out-of-plane component of the M _T for an increasing external field.

To obtain a quantitative insight into the tip magnetization M _T, we apply a Stoner-Wohlfarth (SW) model [55] (Fig. 7d) to the dI/dV hysteresis in Fig. 7c. The SW-model employs two angles α and θ, which represent the tilting of the magnetic easy axis and of the magnetization vector, respectively, from the axis of the external field. The field-dependence of the magnetization in the SW-model is described by the equation

$$h\left( m \right) = - \frac{{Am\sqrt {1 - m^{2} } + B\left( {1 - 2m^{2} } \right)}}{{\sqrt {1 - m^{2} } }},$$

(9)

where A = cos ²α − sin ²α and B = cosα·sinα. Here the reduced magnetization m ≡ M/M _sat = cosθ and the reduced external magnetic field h ≡ μ ₀ M _sat VH/2K _a, where M _sat, V, and K _a represent the saturation magnetization, particle volume, and magnetic anisotropy constant, respectively, are used. The fit of the dI/dV hysteresis in Fig. 7c to Eq. 9 (dotted curves with dotted arrows) results in α = 55 ± 1°. This implies that M _T is tilted by 55 ± 1° at zero-field, away from the sample normal, as shown schematically in Fig. 7d.

Spin-stm with quantitatively characterized magnetic tips

In this section, we introduce some recent applications of spin-STM to unravel non-collinear spin ordering and spin-dependent electronic structures in nanometer scale magnetic structures, based on the quantitative characterizations of tips as discussed in the last section.

Non-collinear spin order probed by field-tuned tips

Experimental proof of noncollineartiy of a periodic spin-dependent dI/dV pattern

A spatially periodic magnetic state could originate from either a collinear [56, 57] or non-collinear [9] spin-density wave (SDW). A collinear-SDW is characterized by a periodic change of the magnitude of the spin moments, while the spin orientation is fixed. On the other hand, a non-collinear SDW is composed of spin moments of constant magnitude but with changing orientation. The dI/dV signal in spin-STS depends on $\hat{\varvec{e}}_{\text{T}} \cdot \hat{\varvec{e}}_{\text{S}}$ (Eq. 7) [15]. If one uses a tip of in-plane oriented M _T at zero field, as induced by an in-plane magnetic anisotropy, the tip is sensitive only to the in-plane component of M _S (M _S,||) at zero field. On the other hand, the tip will be sensitive only to the out-of-plane component of M _S ($M_{{{\text{S}},{ \bot }}}$) at a field large enough to saturate M _T along the field direction. Accordingly, magnetic-field-dependent dI/dV measurement for a collinear-SDW will result only in a change of magnitude, but not of the phase, with changing field. In contrast, measurement of a non-collinear SDW with the same tip will show a field-dependent phase shift of the stripe pattern of the dI/dV signal, since the tip gets more sensitive to $M_{{{\text{S}},{ \bot }}}$ as the field increases [9].

Revealing noncollinearity of stripe patterns in BLH Fe nanoisland

Figure 8a, b show CC-STM and dI/dV images of a Fe|Co island, measured at 0 T. Figure 8c is a hard sphere model representing the atomic stacking in Fe region 1 of b. The Fe regions at the three corners of the island show a stripe contrast along three different directions as indicated by the solid lines superposed along the stripes with the labels 1–3. To resolve the spin ordering in the stripe patterns, we perform in-field spin-STS with the SW tip as characterized by spin-STM on a BLH Co on Cu(111) (Fig. 7). In this tip the direction of M _T is tuned by an external field. The magnetic easy axis of the tip is canted by 55 ± 1° from the sample normal. Therefore, it is sensitive to both $M_{{{\text{S}},{ \bot }}}$ M _T,|| and $M_{{{\text{S}},{ \bot }}}$ at 0 T, while it is sensitive only to the $M_{{{\text{S}},{ \bot }}}$ at a field large enough to saturate $M_{{{\text{S}},{ \bot }}}$. Figure 8d shows the field dependence of the dI/dV profile along the line AA’ perpendicular to the stripe direction of region 1 in Fig. 8b. The wavelength of the stripe pattern, as denoted, is identical with that (1.28 nm) observed in the pure Fe island [7, 20]. Figure 8e shows a zoom-in of the field dependence between two maxima in the profiles, as shown within the grey dashed line in Fig. 8d, for clarity. With increasing magnetic field, the positions of maxima and minima move monotonically from right to left, while the distance between the extrema remains constant. A phase shift of ∆P ~ 0.18 nm is measured upon a change of the magnetic field from 0 to 1.5 T. This observation rules out a collinear SDW. Rather, in-field spin-STS identifies a non-collinear-SDW as the spin texture of the stripe contrast.

Simulation of phase shift in the field dependence of the stripe pattern

Based on Wortmann et al.’s discussion [15], the dI/dV|_mag (Eq. 7) signal is proportional to the projection of M _S to M _T at the tip position, i.e., $\hat{\varvec{e}}_{\text{T}} \cdot \hat{\varvec{e}}_{\text{S}}$. Here we calculate a normalized $\varvec{M}_{\text{T}} \cdot \varvec{M}_{\text{S}}$ ($\left. {\varvec{M}_{\text{T}} \cdot \varvec{M}_{\text{S}} } \right|_{\text{norm}}$) with respect to the external field. We model M _T as a SW magnet of a magnetic easy axis canted by α = 55° from the external field direction, as discussed in Fig. 7c and d. An ab initio study of the sample configuration [7] predicted a Néel-type non-collinearity, where the plane of the spin rotation is parallel with the wave vector of a periodicity λ _SH = 1.28 nm. Thereby, we call this spin order a “spin-cycloid” in the rest of the paper. Then both the out-of-plane (M _S,z) and in-plane (M _S,x) components of the M _S show a sinusoidal position dependence along the x-axis. Thus, $\hat{\varvec{e}}_{{\text{S,z}}}$ and $\hat{\varvec{e}}_{{\text{S,x}}}$ can be described by the equations

$$\hat{\varvec{e}}_{{\text{S,z}}} = \sin \left( {\frac{2\pi x}{{\lambda_{\text{SH}} }}} \right),\quad\hat{\varvec{e}}_{{\text{S,x}}} = \sin \left( {\frac{2\pi x}{{\lambda_{\text{SH}} }} \mp \frac{\pi }{2}} \right),$$

(10)

where the signs ‘−’ and ‘+’ in the formula of $\hat{\varvec{e}}_{{\text{S,x}}}$ indicate a right-rotating (RR) and left- rotating (LR) cycloid, respectively.

We calculate the signal induced by the stripe pattern in region 1 in Fig. 8b. Figure 9a shows a description of M _T, with the polar (θ _T) and azimuthal (φ _T) angles, in the Cartesian coordinate system. A sketch of the geometric relation between the in-plane component of the tip magnetization M _T,|| and the wave vector k ₁ of the stripe pattern for region 1 in Fig. 8b is presented. Figure 9b shows the field dependence $\left. {\varvec{M}_{\text{T}} \cdot \varvec{M}_{\text{S}} } \right|_{\text{norm}}$ as a function of position x (lower figure), calculated with α = 55° and φ _T = 170° for a RR-cycloid, with the x-position dependent out-of-plane (black dotted) and in-plane (red dotted) components of M _S(x) (upper figure). Figure 9c shows the results of the corresponding calculation but for a LR-cycloid. Note the left-to-right (right-to-left) shift of the maxima of $\left. {\varvec{M}_{\text{T}} \cdot \varvec{M}_{\text{S}} } \right|_{\text{norm}}$ from 0 to 1.5 T for the RR- (LR-) cycloid for the given azimuthal angle of M _T. For the stripe contrast in region 1 of the island in Fig. 8, we observe that the extrema of the dI/dV curves shift from right to left. Interestingly, the three cases show different amounts of phase shifts with increasing field (Supplementary Information of [7]). We perform a quantitative analysis of the phase shift and its dependence on stripe orientation and field. An excellent agreement between the experiments and simulations reveals that the field dependence of the phase shifts is determined by a given orientation of the tip magnetization.

Spin-STM of a non-collinear magnetic state with a superparamagnetic tip

Figure 10a is CC-STM image of a BLH Fe island on Cu(111) in bridge-site stacking of the topmost atoms, measured with a Fe-coated W tip. Figures 10b–d are dI/dV images of the same island as that of Fig. 10a measured at 0 T, +1.5 T, and −1.5 T, respectively. The stripe patterns in Fig. 10c, d indicate a cycloidal spin order as discussed in the text above describing Figs. 8 and 9. However, no stripe contrast is observed in the dI/dV map at zero field. We obtained dI/dV images under an external field from −3 to +3 T along the sample normal. We show in Fig. 10e the stripe contrast at 5 field values, measured along a direction perpendicular to the stripe patterns as indicated by the white lines in Fig. 10b–d. Figure 10f shows the field dependence of the stripe contrast (red), peak-to-peak amplitude of the contrast oscillation at each field followed by a normalization with the saturation value from the Langevin fitting (Eq. 8). The inspection of Fig. 10e reveals two aspects: (1) The contrast at a given position increases for increasing applied field. No stripe contrast is observed at zero field. The stripe contrast saturates at ~±1.5 T. (2) The contrast depends only on the magnitude of the field, but not on the sign of the field. The extrema positions of the stripe patterns as indicated by the yellow and blue dashed lines in Fig. 10c and d remain unchanged. To obtain a quantitative insight into the field dependence of the stripe contrast (red curve in Fig. 10f), we also obtained the field dependence of dI/dV signals measured at the center of the Co core of a Fe|Co island (inset) with the same tip. This measurement on the Co reference sample definitely reflects the response of the tip to the applied field (blue in Fig. 10f). This tip behaves as a superparamagnetic particle. The larger slope near zero field for measurements on Co (blue curve) as compared to measurements on Fe (red curve), clearly implies a sizable contribution of the response of the sample magnetic order to the measured quantity of the dI/dV signal (red). In addition, the results imply a ‘non-hysteretic’ and ‘monotonic’ response of the Fe magnetic order to the applied field.

The field dependence of the magnetization M _T of a superparamagnetic tip can be written as M _T(H) = −M _T(−H) (blue curve in Fig. 10f). The field dependence of the dI/dV signal of the pure Fe island shown in Fig. 10 reveals a relation of dI/dV (−H) = dI/dV (H) (red). Then, the relation given by Wortmann et al., dI/dV|_mag = m _T · m _Fe, resolves the influence of the sign reversal in H on the magnetization density of state m _Fe (see Sect. 1.2) through a simple calculation

$$\left. {\frac{dI}{dV}\left( { - H} \right)} \right|_{\text{mag}} = \varvec{m}_{\text{T}} \left( { - H} \right) \cdot \varvec{m}_{\text{Fe}} \left( { - H} \right) \Leftrightarrow \left. {\frac{dI}{dV}\left( H \right)} \right|_{\text{mag}} = \varvec{m}_{\text{T}} \left( H \right) \cdot \varvec{m}_{\text{Fe}} \left( H \right),$$

(11)

which leads to a relation m _S(−H _ext) = −m _S(H _ext). This, concurrent with the above-mentioned ‘non-hysteretic’ and ‘monotonic’ field dependence, provides an important conclusion on the magnetic property of the non-collinear spin order in the Fe island. The stripe order in Fe island responds to the external field as an effective magnetic moment, which is thermally fluctuating at a given measurement temperature. We show in the next section the significance of this aspect to obtain a spin-polarization map of the Fe stripe phase from the data set shown in Fig. 10a–c.

Spin-polarization of magnetically ordered nanostructures

Differential conductance asymmetry

The magnetic configuration of a sample is determined by its spin-dependent electronic structure, giving rise to spin polarization of the electronic density of states. To investigate the spin polarization of a sample with spin-STM, the asymmetry of the differential conductance, A _dI/dV, is introduced. The asymmetry is defined as [5]

$$A_{{{\text{dI}}/{\text{dV}}}} = \frac{{\left. {{\text{d}}I/{\text{d}}V} \right|_{\text{AP}} - \left. {{\text{d}}I/{\text{d}}V} \right|_{\text{P}} }}{{\left. {{\text{d}}I/{\text{d}}V} \right|_{\text{AP}} + \left. {{\text{d}}I/{\text{d}}V} \right|_{\text{P}} }}$$

(12)

In case of a ferromagnetic sample of bistable magnetization, A _dI/dV is calculated from the dI/dV signals recorded under P and AP to the unit vector of magnetization configurations, i.e. ê _T·ê _S = ±1, as schematically illustrated in Fig. 11a. As introduced in Sect. 1.2, Wortmann et al. derived the description of the dI/dV signal measured by spin-STM [15] (Eq. 7). Substitution of their result into the Eq. 12 leads to

$$A_{{{\text{dI}}/{\text{dV}}}} = - P_{\text{T}} P_{\text{S}} ,$$

(13)

which links the dI/dV asymmetry, A _dI/dV, to the spin polarization of the sample at the tip apex position, P _S(R _T).

Equations 11 and 12 were applied to the Co island ‘A’ in Fig. 5a to extract the spatial distribution of its spin-polarization. Figure 11a, b are two dI/dV images on the island measured at μ₀ H = −1.1 T, with (b) AP and (c) P magnetization configurations, as indicated in Fig. 5c. Figure 11d is the A _dI/dV map, at the given bias voltage V _b, calculated from the dI/dV images in Fig. 11b and c. Oka et al. extracted a set of energy-resolved A _dI/dV maps of this Co island, which led to the disclosure of the electronic nature of “spin-dependent quantum interference within a single nanostructure” [5].

Differential conductance asymmetry of non-collinear magnetic order

In case of a helical (or cycloidal) spin order, the local magnetization rotates with a spatial period. Thus, the spatially averaged magnetization is zero. As discussed in Sect. 4.2, a sign reversal of the external field induces a corresponding reversal in that of the local magnetization, M _S(r; −H) = −M _S(r; H), indicative of two distinct antiparallel magnetic states at each position r. In addition, the power of spin-STM, which allows to resolve the local magnetic signal down to the atomic scale, makes a study on the local spin-polarization of the cycloidal order in the bilayer Fe island feasible. Although the definition of AP and P configurations is not applicable to this case due to the periodic change of the local magnetization, one can clearly distinguish two distinct magnetic states, as sketched in Fig. 11e. Combined with the tip magnetic state, we introduce two magnetic configurations α and β, hence M _S,(r) = −M _S,β(r), analogous to the AP and P configurations in the case of Fig. 11a. The asymmetry A _dI/dV for the cycloidal spin order in the Fe island is defined as

$$A_{{{\text{dI}}/{\text{dV}}}} = \frac{{\left. {{\text{d}}I/{\text{d}}V} \right|_{\alpha } - \left. {{\text{d}}I/{\text{d}}V} \right|_{\beta } }}{{\left. {{\text{d}}I/{\text{d}}V} \right|_{\alpha } + \left. {{\text{d}}I/{\text{d}}V} \right|_{\beta } }}$$

(14)

With substitution of the Eqs. 7, 14 becomes

$$A_{{{\text{dI}}/{\text{dV}}}} = \frac{{n_{\text{T}} n_{\text{S}} + \varvec{m}_{\text{T}} \cdot \varvec{m}_{{{\text{S}},\alpha }} - n_{\text{T}} n_{\text{S}} - \varvec{m}_{\text{T}} \cdot \varvec{m}_{{{\text{S}},\beta }} }}{{n_{\text{T}} n_{\text{S}} + \varvec{m}_{\text{T}} \cdot \varvec{m}_{{{\text{S}},\alpha }} + n_{\text{T}} n_{\text{S}} + \varvec{m}_{\text{T}} \cdot \varvec{m}_{{{\text{S}},\beta }} }} = - \frac{{\varvec{m}_{\text{T}} \cdot \varvec{m}_{{{\text{S}},\alpha }} }}{{n_{\text{T}} n_{\text{S}} }}$$

(15)

This leads to a link between the symmetry A _dI/dV and the spin polarization of the sample at the tip apex position, P _S(R _T) in the form

$$A_{{{\text{dI}}/{\text{dV}}}} = - P_{\text{T}} P_{\text{S}} \left( {\varvec{R}_{\text{T}} } \right)\cos \theta ,$$

(16)

where θ is the angle between M _T and M _S (see Fig. 1a). The asymmetry A _dI/dV corresponds to the projection of P _S onto the tip magnetization direction.

If a superparamagnetic tip (Fig. 6) is used in spin-STM/S of the cycloidal spin order in the bilayer Fe island, one is not able to have the above-mentioned two magnetization configurations (α and β) because the tip magnetization will also be reversed by the sign reversal of the applied field, as discussed in Fig. 10. This always results in the numerator of the Eq. (14) to be zero. We introduce a procedure to overcome this obstacle in the following discussion. A careful inspection of the right hand side of Eq. 15 indicates that the denominator and numerator are no other than non-magnetic and magnetic terms of the dI/dV signals for the configuration α, respectively. These two contributions are provided by the dI/dV|_H=0 and dI/dV|_α – dI/dV|_H=0 data, respectively. Figure 11f, g show the dI/dV|_H=0 and dI/dV|_α maps of a bilayer Fe nanoisland measured with a superparamagnetic tip, and Fig. 11h is its A _dI/dV map, derived from Fig. 11f and g as given by Eq. 15. Fischer et al. extracted a set of energy-resolved A _dI/dV maps of this Fe island, which were successfully utilized to reveal the “spinor nature of electronic states in nanosize non-collinear magnets” [20].

Concluding remarks

In the recent two decades, spin-STM has evolved into a reliable and versatile tool for spatial mapping of local magnetic structures of collinear and non-collinear spin textures on the nano-scale. The unsurpassed lateral resolution turned spin-STM into a unique tool to collect the magnetic information down to the atomic scale of single nanostructures. The tunneling nature of STM/S inevitably couples contributions from both tip and sample in the measured signals, I(V) and dI/dV(V). Understanding the tip contribution has been a challenging issue for a reliable analysis of the sample properties. Undoubtedly, this is also true in the spin-STM/S measurements. In this review, we introduced some examples of tip characterization in spin-STM/S experiments. This analysis has advanced the quantitative physical understanding of spin textures in nanostructures.

Based on in situ reference measurements on the bistable out-of-plane magnetization of biatomic-layer-high Co nanoislands on Cu (111), we characterized magnetic states of spin-STM tips quantitatively. Temperature-dependent in-field spin-STM/S gives a quantitative characterization of tips in the superparamagnetic state. The analysis reveals stray field at the tip position induced by the sample magnetization. In-field spin-STM/S combined with the Stoner-Wohlfarth (SW) model [55] for tip magnetization elucidates the orientation of the magnetic anisotropy of bistable ferromagnetic tips. Our studies show that the SW model within the framework of the superparamagnetic criterion indeed explains the magnetic response of tips of various types, which give rise to distinctly different field-dependence of the spin-STS signal.

In-field STM/S in combination, such sophisticated tip characterization allows to characterize the local magnetic order and local spin-dependent electronic structure of magnetic nanostructures. Field-tuning of the orientation of a magnetically bistable tip was applied to reveal the non-collinearity of the one-dimensional periodic magnetic order in Fe nanoislands. The spin-dependent dI/dV mapping of Co and Fe nanostructures, in antiparallel and parallel configurations of tip and sample magnetizations, provides differential conductance asymmetry maps, which directly link spin-STS data to the local spin-polarization within a single nanostructure.

In spite of the remarkable advances to date in the characterization of the tip states by exploiting external field control, the spin-STM research field still requires more effort to overcome the following existing barriers. It is a goal to define the tip apex to maintain a specific structural configuration on the atomic scale during a set of measurements over periods ranging from days to months. However, a specific recipe of macroscopic (or ex situ) tip preparation does not seem to play a decisive role for the resulting magnetic behavior, as we demonstrated in this review (Fig. 4). Up to now, preparation and tuning of a tip is extremely tricky. Key ingredients are in situ treatments by voltage pulses. The tip never comes back to its original form once the tip loses its microscopic configuration by crashes with the sample, which is unfortunately common in STM measurement. Manipulation technique of single atoms on a surface using STM tips [10, 58–61] has been advanced significantly through precise estimation of the force required to move an individual atom on a surface [62, 63]. This allows to reliably attach/detach individual atoms to/from the tip apex without any change of the rest of the tip. In addition, complete control of the vector nature of the tip and sample magnetizations call for a “vector magnet field”, which comes with a high price tag. Future advance in spin-STM is guaranteed by the combination of these advanced techniques.

References

1.
M. Bode, Spin-polarized scanning tunnelling microscopy. Rep. Prog. Phys. 66, 523 (2003)
Article Google Scholar
2.
W. Wulfhekel, J. Kirschner, Spin-polarized scanning tunneling microscopy of magnetic structures and antiferromagnetic thin films. Annu. Rev. Mater. Res. 37, 69 (2007)
Article Google Scholar
3.
R. Wiesendanger, Spin mapping at the nanoscale and atomic scale. Rev. Mod. Phys. 81, 1495 (2009)
Article Google Scholar
4.
H. Oka, O.O. Brovko, M. Corbetta, V.S. Stepanyuk, D. Sander, J. Kirschner, Spin-polarized quantum confinement in nanostructures: scanning tunneling microscopy. Rev. Mod. Phys. 86, 1127–1168 (2014)
Article Google Scholar
5.
H. Oka, P.A. Ignatiev, S. Wedekind, G. Rodary, L. Niebergall, V.S. Stepanyuk, D. Sander, J. Kirschner, Spin-dependent quantum interference within a single magnetic nanostructure. Science 327, 843 (2010)
Article Google Scholar
6.
S. Ouazi, S. Wedekind, G. Rodary, H. Oka, D. Sander, J. Kirschner, Magnetization reversal of individual co nanoislands. Phys. Rev. Lett. 108, 107206 (2012)
Article Google Scholar
7.
S.H. Phark, J.A. Fischer, M. Corbetta, D. Sander, K. Nakamura, J. Kirschner, Reduced-dimensionality-induced helimagnetism in iron nanoislands. Nat. Commun. 5, 5183 (2014)
Article Google Scholar
8.
S. Heinze, M. Bode, A. Kubetzka, O. Pietzsch, X. Nie, S. Blügel, R. Wiesendanger, Real-space imaging of two-dimensional antiferromagnetism on the atomic scale. Science 288, 1805 (2000)
Article Google Scholar
9.
M. Bode et al., Chiral magnetic order at surfaces driven by inversion asymmetry. Nature 447, 190–193 (2007)
Article Google Scholar
10.
S. Loth, S. Baumann, C.P. Lutz, D.M. Eigler, A.J. Heinrich, Bistability in atomic-scale antiferromagnets. Science 335, 196–199 (2012)
Article Google Scholar
11.
P.M. Tedrow, R. Meservey, Spin polarization of electrons tunneling from films of Fe Co, Ni, and Gd. Phys. Rev. B 7, 318 (1973)
Article Google Scholar
12.
R. Meservey, P.M. Tedrow, P. Fulde, Magnetic field splitting of the quasiparticle states in superconducting aluminum films. Phys. Rev. Lett. 25, 1270 (1970)
Article Google Scholar
13.
M. Julliere, Tunneling between ferromagnetic films. Phys. Lett. 54A, 225 (1975)
Article Google Scholar
14.
C. Kittel, Physical theory of ferromagnetic domains. Rev. Mod. Phys. 21, 541 (1949)
Article Google Scholar
15.
D. Wortmann, S. Heinze, P. Kurz, G. Bihlmayer, S. Blügel, Resolving complex atomic-scale spin structures by spin-polarized scanning tunneling microscopy. Phys. Rev. Lett. 86, 4132 (2001)
Article Google Scholar
16.
J. Bardeen, Tunneling from a many-particle point of view. Phys. Rev. Lett. 6, 57–59 (1961)
Article Google Scholar
17.
J. Tersoff, D.R. Hamann, Theory of the scanning tunneling microscope. Phys. Rev. B 31, 805 (1985)
Article Google Scholar
18.
D. Sander, S.H. Phark, M. Corbetta, J.A. Fischer, H. Oka, J. Kirschner, The impact of structural relaxation on spin polarization and magnetization reversal of individual nano structures studied by spin-polarized scanning tunneling microscopy. J. Phys.: Condens. Matter 26, 394008 (2014)
Google Scholar
19.
S.H. Phark, J.A. Fischer, M. Corbetta, D. Sander, J. Kirschner, Superparamagnetic response of Fe-coated W tips in spin-polarized scanning tunneling microscopy. Appl. Phys. Lett. 103, 032407 (2013)
Article Google Scholar
20.
J.A. Fischer, L.M. Sandratskii, S.H. Phark, S. Ouazi, A.A. Pasa, D. Sander, S.S.P. Parkin, Probing the spinor nature of electronic states in nanosize non-collinear magnets. Nat. Commun. (2016). doi:10.1038/ncomms13000
Google Scholar
21.
M.F. Crommie, C.P. Lutz, D.M. Eigler, Imaging standing waves in a two-dimensional electron gas. Nature (London) 363, 524 (1993)
Article Google Scholar
22.
L. Diekhöner, M.A. Schneider, A.N. Baranov, V.S. Stepanyuk, P. Bruno, K. Kern, Surface states of cobalt nanoislands on Cu(111). Phys. Rev. Lett. 90, 236801 (2003)
Article Google Scholar
23.
A. Biedermann, W. Rupp, M. Schmid, P. Varga, Coexistence of fcc- and bcc-like crystal structures in ultrathin Fe films grown on Cu(111). Phys. Rev. B 73, 165418 (2006)
Article Google Scholar
24.
L. Gerhard et al., Magnetoelectric coupling at metal surfaces. Nat Nanotech. 5, 792–797 (2010)
Article Google Scholar
25.
G. Rodary, S. Wedekind, H. Oka, D. Sander, J. Kirschner, Characterization of tips for spin-polarized scanning tunneling microscopy. Appl. Phys. Lett. 95, 152513 (2009)
Article Google Scholar
26.
M. Corbetta, S. Ouazi, J. Borme, Y. Nahas, F. Donati, H. Oka, S. Wedekind, D. Sander, J. Kirschner, Magnetic response and spin polarization of bulk Cr tips for in-field spin-polarized scanning tunneling microscopy. Jpn. J. Appl. Phys. 51, 208 (2012)
Article Google Scholar
27.
S. Maekawa, U. Gäfvert, Electron tunneling between ferromagnetic films. IEEE Trans. Magn. 18, 707 (1982)
Article Google Scholar
28.
T. Miyazaki, N. Tezuka, Giant magnetic tunneling effect in Fe/Al2O3/Fe junction. J. Magn. Magn. Mater. 139, L231 (1995)
Article Google Scholar
29.
J.S. Moodera, L.R. Kinder, T.M. Wong, R. Meservey, Large magnetoresistance at room temperature in ferromagnetic thin film tunnel junctions. Phys. Rev. Lett. 74, 3273 (1995)
Article Google Scholar
30.
M.W.J. Prins, D.L. Abraham, H. van Kempen, Spin-dependent transmission at ferromagnet/semiconductor interfaces. J. Magn. Magn. Mater. 121, 152 (1993)
Article Google Scholar
31.
P.M. Tedrow, R. Meservey, Direct observation of spin-state mixing in superconductors. Phys. Rev. Lett. 27, 919 (1971)
Article Google Scholar
32.
P.M. Tedrow, R. Meservey, Spin-dependent tunneling into ferromagnetic nickel. Phys. Rev. Lett. 26, 192 (1971)
Article Google Scholar
33.
W. Wulfhekel, J. Kirschner, Spin-polarized scanning tunneling microscopy on ferromagnets. Appl. Phys. Lett. 75, 1944–1946 (1999)
Article Google Scholar
34.
C.L. Gao, U. Schlickum, W. Wulfhekel, J. Kirschner, Mapping the surface spin structure of large unit cells: reconstructed Mn films on Fe(001). Phys. Rev. Lett. 98, 107203 (2007)
Article Google Scholar
35.
K. von Bergmann, M. Menzel, D. Serrate, Y. Yoshida, S. Schröder, P. Ferriani, A. Kubetzka, R. Wiesendanger, S. Heinze, Tunneling anisotropic magnetoresistance on the atomic scale. Phys. Rev. B 86, 134422 (2012)
Article Google Scholar
36.
N. Néel, S. Schröder, N. Ruppelt, P. Ferriani, J. Kröger, R. Berndt, S. Heinze, Tunneling tunneling anisotropic magnetoresistance on the atomic scale. Phys. Rev. Lett. 110, 037202 (2013)
Article Google Scholar
37.
N.M. Caffrey, S. Schröder, S.Heinze Ferriani, Tunneling anisotropic magnetoresistance effect of single adatoms on a noncollinear magnetic surface. J. Phys.: Condens. Matter 26, 394010 (2014)
Google Scholar
38.
M. Cavallini, F. Biscarini, Electrochemically etched nickel tips for spin polarized scanning tunneling microscopy. Rev. Sci. Instr. 71, 4457–4460 (2000)
Article Google Scholar
39.
A.L. Bassi, C.S. Casari, D. Cattaneo, F. Donati, S. Foglio, M. Passoni, C.E. Bottani, P. Biagioni, A. Brambilla, M. Finazzi, F. Ciccacci, L. Duò, Appl. Phys. Lett. 91, 173120 (2007)
Article Google Scholar
40.
A.A. Minakov, I.V. Shvets, On the possibility of resolving quantization axes of surface spins by means of a scanning tunneling microscope with a magnetic tip. Surf. Sci. 236, L377–L381 (1990)
Article Google Scholar
41.
S. Murphy, J. Osing, I.V. Shvets, Fabrication of submicron-scale manganese-nickel tips for spin-polarized STM studies. Appl. Surf. Sci. 144–145, 497–500 (1999)
Article Google Scholar
42.
G. Mariotto, S. Murphy, I.V. Shvets, Charge ordering on the surface of Fe3O4(001). Phys. Rev. B 66, 245426 (2002)
Article Google Scholar
43.
S.F. Ceballos, G. Mariotto, S. Murphy IV, I.V. Shvets, Fabrication of magnetic STM probes and their application to studies of the Fe3O4(001) surface. Surf. Sci. 523, 131–140 (2003)
Article Google Scholar
44.
T.E. Feuchtwang, P.H. Cutler, J. Schmit, Surf. Sci. 75, 401 (1978)
Article Google Scholar
45.
S. Nagai, K. Hata, H. Oka, D. Sander, J. Kirschner, Atomic structure and spin polarization at the apex of tips used in spin-polarized scanning tunneling microscopy. Appl. Phys. Exp. 7, 025204 (2014)
Article Google Scholar
46.
T. Hashizume, Y. Hasegawa, I. Kamiya, T. Ide, I. Sumita, S. Hyodo, T. Sakurai, H. Tochihara, M. Kubota, Y. Murata, J. Vac. Sci. Technol., A 8, 233 (1990)
Article Google Scholar
47.
O. Pietzsch, A. Kubetzka, M. Bode, R. Wiesendanger, Spin-polarized scanning tunneling spectroscopy of nanoscale cobalt islands on Cu(111). Phys. Rev. Lett. 92, 057202 (2004)
Article Google Scholar
48.
Y. Yayon, V.W. Brar, L. Senapati, S.C. Erwin, M.F. Crommie, Observing spin polarization of individual magnetic adatoms. Phys. Rev. Lett. 99, 067202 (2007)
Article Google Scholar
49.
C. Iacovita, M.V. Rastei, B.W. Heinrich, T. Brumme, J. Kortus, L. Limot, J.P. Bucher, Visualizing the spin of individual cobalt-phthalocyanine molecules. Phys. Rev. Lett. 101, 116602 (2008)
Article Google Scholar
50.
J. de la Figuera, J.E. Prieto, C. Ocal, R. Miranda, Scanning-tunneling-microscopy study of the growth of cobalt on Cu(111). Phys. Rev. B 47, 13043(R) (1993)
Article Google Scholar
51.
N.N. Negulyaev, V.S. Stepanyuk, P. Bruno, L. Diekhöner, P. Wahl, K. Kern, Bilayer growth of nanoscale Co islands on Cu(111). Phys. Rev. B 77, 125437 (2008)
Article Google Scholar
52.
C.P. Bean, J.D. Livingston, Superparamagnetism. J. Appl. Phys. 30, S120 (1959)
Article Google Scholar
53.
I.M.L. Billas, J.A. Becker, A. Chârelain, W.A. de Heer, Magnetic moments of iron clusters with 25 to 700 atoms and their dependence on temperature. Phys. Rev. Lett. 71, 4067 (1993)
Article Google Scholar
54.
M.B. Stearns, Magnetic properties of 3d, 4d, and 5d elements alloys and compounds (Landolt-Bornstein numerical data and functional relationships in science and technology group III) (Springer, Berlin, 1986)
Google Scholar
55.
E. Stoner, E. Wohlfarth, A mechanism of magnetic hysteresis in heterogeneous alloys. Philos Trans R Soc A Phys Mech Eng Sci 240, 599–642 (1948)
Article Google Scholar
56.
A.W. Overhauser, Spin density waves in an electron gas. Phys. Rev. 128, 1437–1452 (1962)
Article Google Scholar
57.
E. Fawcett, Spin-density-wave antiferromagnetism in chromium. Rev. Mod. Phys. 60, 209–283 (1988)
Article Google Scholar
58.
M.F. Crommie, C.P. Lutz, D.M. Eigler, Confinement of electrons to quantum corrals on a metal surface. Science 262, 218–220 (1993)
Article Google Scholar
59.
H.C. Manoharan, C.P. Lutz, D.M. Eigler, Quantum mirages formed by coherent projection of electronic structure. Nature 403, 512–515 (2000)
Article Google Scholar
60.
A.J. Heinrich, C.P. Lutz, J.A. Gupta, D.M. Eigler, Molecule cascades. Science 298, 1381–1387 (2002)
Article Google Scholar
61.
C.F. Hirjibehedin, C.P. Lutz, A.J. Heinrich, Spin coupling in engineered atomic structures. Science 312, 1021–1024 (2006)
Article Google Scholar
62.
M. Ternes, C.P. Lutz, C.F. Hirjibehedin, F.J. Giessibl, A.J. Heinrich, The force needed to move an atom on a surface. Science 319, 1066–1069 (2008)
Article Google Scholar
63.
M. Ternes, C. González, C.P. Lutz, P. Hapala, F.J. Giessibl, P. Jelínek, A.J. Heinrich, Interplay of conductance, force, and structural change in metallic point contacts. Phys. Rev. Lett. 106, 016802 (2011)
Article Google Scholar
64.
S. Chikazumi, Physics of ferromagnetism, international series of monographs on physics, 2nd edn. (Oxford University Press, New York, 1997)
Google Scholar

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Authors’ contributions

SHP and DS conceived and designed the contents of the paper. All authors discussed and wrote the paper. Both authors read and approved the final manuscript.

Acknowledgements

S. Phark acknowledges support from IBS-R027-D1. D. Sander acknowledges partial financial support by DFG SFB762. All the experiments were performed using the low-temperature STM of the Max-Planck-Institute of Microstructure Physics at Halle, Germany. S. Phark heartfully thanks Y. J. Chang and A. J. Heinrich for careful reading, sophisticated discussion, and useful corrections of the manuscript.

Competing interests

The authors declare that they have no competing interests.

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The datasets supporting the conclusions of this article are included within the article.

Funding

DFG SFB762 partially supports the design and experiments of the study in the manuscript. IBS-R027-D1 supports the interpretation of data and writing process of the manuscript.

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Center for Quantum Nanoscience, Institute for Basic Science, Seoul, 03760, Republic of Korea
Soo-hyon Phark
Department of Physics, Ewha Womans University, Seoul, 03760, Republic of Korea
Soo-hyon Phark
Max-Planck-Institut für Mikrostrukturphysik, 06120, Halle, Germany
Dirk Sander

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Phark, S., Sander, D. Spin-polarized scanning tunneling microscopy with quantitative insights into magnetic probes. Nano Convergence 4, 8 (2017). https://doi.org/10.1186/s40580-017-0102-5

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Received: 07 February 2017
Accepted: 29 March 2017
Published: 06 April 2017
DOI: https://doi.org/10.1186/s40580-017-0102-5

Keywords

Spin-polarized scanning tunneling microscopy
Nanomagnetism
Magnetic anisotropy
Non-collinear magnetic order