Abstract
Chiral spin textures of a ferromagnetic layer in contact to a heavy nonmagnetic metal, such as Néeltype domain walls and skyrmions, have been studied intensively because of their potential for future nanomagnetic devices. The Dyzaloshinskii–Moriya interaction (DMI) is an essential phenomenon for the formation of such chiral spin textures. In spite of recent theoretical progress aiming at understanding the microscopic origin of the DMI, an experimental investigation unravelling the physics at stake is still required. Here we experimentally demonstrate the close correlation of the DMI with the anisotropy of the orbital magnetic moment and with the magnetic dipole moment of the ferromagnetic metal in addition to Heisenberg exchange. The density functional theory and the tightbinding model calculations reveal that inversion symmetry breaking with spin–orbit coupling gives rise to the orbitalrelated correlation. Our study provides the experimental connection between the orbital physics and the spin–orbitrelated phenomena, such as DMI.
Introduction
Chiral interaction between two atomic spins owing to a strong spin–orbit coupling (SOC), which is known as the Dzyaloshinskii–Moriya interaction (DMI), has attracted intense interest^{1,2}. In particular, it has been demonstrated that the DMI at the interface between ferromagnetic (FM) and nonmagnetic heavy metals (HMs) plays a major role for the formation of chiral spin textures, such as skyrmions^{3,4} and homochiral Néeltype domain walls (DWs)^{5,6,7}, which are attractive for the development of future information storage technology^{8}. Understanding the microscopic origin of the DMI is indispensable for the realization of such chiral spin textures^{9,10}. It has been reported that the proximityinduced magnetic moment in HM layers is critical to promote the DMI^{11}. However, this proximity effect is still controversial because it has been also reported that the induced magnetic moment has no direct correlation with the DMI in the case of the Co/Pt system^{12,13}. The scattering of spinpolarized electrons on spin–orbit coupled impurities is known to give rise to the DMI in spinglass systems as a microscopic viewpoint^{14,15}. However, the orbital hybridization between the spin–orbit coupled ions and the magnetic matrix was explicitly neglected in the theory, which becomes problematic when considering transition metal interfaces. On the other hand, theories have predicted that SOC combined with inversion symmetry breaking (ISB) naturally introduces a chirality to conduction electron spins in equilibrium and the interfacial DMI at an FM/HM interface is related to this spin chirality^{16,17,18,19,20}. It has also been reported that the spin chirality is a manifestation of the chirality of the orbital magnetism in strongly spin–orbit coupled systems with ISB^{21,22}. These previous studies suggest a possible microscopic origin of the interfacial DMI, which has remained experimentally unaddressed so far.
Here we discuss the microscopic origin of the interfacial DMI with experimental and theoretical studies as follows: First, we show the temperature dependence of the DMI for a Pt/Co/MgO trilayer, which is one of the standard structures used for the studies of the DMI^{7,12,23}, using the extended droplet model^{24}. We find that the DMI increases with decreasing temperature in a range from 300 to 100 K. In general, the electron–phonon interaction promotes thermally induced hopping between nearest neighbours when increasing the temperature^{25}. As a result, it is expected that the difference between inplane and outofplane hopping energies is reduced upon temperature increase. Therefore, changing the temperature of the system allows for charge redistribution between inplane and outofplane orbitals while preserving the integrity of electronic states of the trilayer unlike other interface control methods such as ion irradiation^{26} or thermal annealing technique^{27}, which may cause a permanent atomic rearrangement and thus induce undesired extrinsic effects. To discuss this temperature dependence of the DMI, that of the spin (m_{s}) and orbital (m_{o}) magnetic moments of Co and Pt is studied by Xray magnetic circular dichroism (XMCD) spectroscopy. We find that m_{s} values of Co and Pt show temperature dependences due to change in Heisenberg exchange. Furthermore, the intraatomic magnetic dipole moment (m_{D}), which is due to the asymmetric spin density distribution (f_{SD})^{28,29}, displays strong temperature dependence, suggesting a sizable modification of the charge distribution between the inplane and the outofplane dorbitals under temperature variation. We also find that the outofplane orbital moment (\({\boldsymbol{m}}_{\mathrm{o}}^ \bot\)) shows large temperature dependence while inplane orbital moment (\({\boldsymbol{m}}_{\mathrm{o}}^\parallel\)) does not, revealing a close connection between the anisotropy of m_{0} (orbital anisotropy) and the DMI. The ab initio and the tightbinding model calculations suggest that the ISBdependent electron hopping, which gives rise to the asymmetric charge distribution at the interface of the FM/HM, is a possible microscopic origin of the correlation between the orbital anisotropy and the DMI.
Results
Temperature dependence of the DMI in the Pt/Co/MgO trilayer
The temperature dependence of the DMIinduced effective field (H_{DMI}) of the Pt (2 nm)/Co (0.5 nm)/MgO (2 nm) trilayer is determined by measuring the nucleation field (H_{n}) applied along the inplane (H_{ x }) and outofplane (H_{ z }) direction as schematically shown in Fig. 1a. The measured H_{n} values are analysed with the extended droplet model^{24}. Since H_{n} is proportional to square of DW energy (\({\mathrm{\sigma }}_{{\mathrm{DW}}}^2\)), the σ_{DW} is a crucial parameter for the nucleation^{24,30}. In case of the droplet with sizable DMI, DW magnetizations are aligned in the radial direction. When we consider the two DW magnetizations with respect to H_{ x }, DW1 and DW2 (see the inset of Fig. 1b), \({\mathrm{\sigma }}_{{\mathrm{DW}}}^2\) of the DW1 and the DW2, respectively, follows the blue and the red curves in terms of H_{ x } due to DMI as illustrated in Fig. 1b^{31}. Assuming that total DW energy mainly depends on the two magnetizations at the DW of a droplet with respect to H_{ x }, the total \({\mathrm{\sigma }}_{{\mathrm{DW}}}^2\) follows the trend of the purpledotted line. Note that there is a threshold where the \({\mathrm{\sigma }}_{{\mathrm{DW}}}^2\) starts to become H_{ x } dependent. Our previous report showed that the extended droplet model allows us to estimate the DMIinduced field from the threshold field^{24}. In spite of such onedimensional approximation, we have demonstrated that the fitting gives reliable value of the DMI energy density (D).
The measured H_{n} as a function of H_{ x } shows a threshold arising from the DMI as predicted by the extended droplet model^{24} (see also Supplementary Note 1, 2 and Method section for details about the analysis and the measurement). Figures 2a–d show H_{n}/H_{SW}(H_{ x }=0) as a function of H_{ x }/H_{ K } at various temperatures (a, T=300 K; b, 200 K; c, 150 K and d, 100 K). Here H_{n} and H_{ x } are normalized by the switching field at H_{ x }=0 [H_{SW}(H_{ x }=0)] and by the anisotropy field (H_{ K }), respectively. Those normalized values allow us to clearly confirm the DMIdependent threshold with ruling out the temperaturedependent characteristics of H_{ K } and the H_{SW}(H_{ x }=0). The temperaturedependent H_{DMI} can be determined from the best fitting using the extended droplet model; H_{DMI} at 300, 200, 150 and 100 K are 166±50, 245±45, 324±15 and 372±30 mT, respectively (Fig. 2e). The temperaturedependent D is readily calculated from H_{DMI} and Δvia \({\boldsymbol{H}}_{{\mathrm{DMI}}} = {\boldsymbol{D}}/\mu _0M_{\mathrm{s}}\varDelta\), where μ_{0} is the permeability, M_{s} is the saturation magnetization and Δ is the DW width^{6}. Δ and M_{s} values in terms of the temperature are listed in Table 1. We find that D has a strong temperature dependence as shown in Fig. 2e; D increases by a factor of 2.2 as the temperature decreases from 300 to 100 K.
Heisenberg exchange is one of key parameters to understand the microscopic origin of DMI^{2,32}. From the temperature dependence of M_{s}, the exchange stiffness constant (A) values were quantitatively obtained as detailed in Supplementary Note 3. As listed in Table 1, we find a clear correlation of the Heisenberg exchange with DMI; the A value increases by 57% when the temperature decreases from 300K to 100 K while DMI shows 100% increase. Based on Moriya’s theory, DMI requires three ingredients: (i) SOC, (ii) magnetic exchange, and (iii) ISB. Therefore, we can consider two parameters in addition to Heisenberg exchange: one is the proximityinduced magnetism of the nonmagnetic element, which is related to the source ii, and the other is the hybridization between 3d and 5d orbitals, which is related to the sources i and iii. In order to find how DMI correlated with the induced moment in the Pt layer and the orbital structure of Co, XMCD studies were performed using the soft and hard Xray as discussed in the following sections.
Temperature dependence of the proximityinduced magnetic moment of Pt
In this section, we first investigate the role of the induced magnetic moment in the Pt layer as mentioned in previous section. The temperature dependence of the Ptinduced magnetic moment was measured using the XMCD method, which enables elementspecific analyses of spin and orbital magnetism^{33,34}. Figure 3a presents the XMCD and integration of XMCD spectra measured at the Pt L_{2,3} edge. The intensities of XMCD are ~3% of the Xray absorption spectra (XAS) edge heights. At both the L_{3} and L_{2} edges (around 11.57 keV and 13.28 keV, respectively), the integrated XMCD spectra show temperature dependences. In contrast, there is no temperature dependence in XAS spectra (see inset of Fig. 3a). The total magnetic moment (m_{total}), which is the sum of an effective spin magnetic moment \(\left( {{\boldsymbol{m}}_{\mathrm{s}}^{{\mathrm{eff}}} = {\boldsymbol{m}}_{\mathrm{s}} + {\boldsymbol{m}}_{\mathrm{D}}} \right)\) and m_{o}, was estimated by a sum rule calculation^{35} (see the details about the sum rule calculation in Supplementary Note 4). In this study, we use moment values per single hole rather than those per atom because it is difficult to precisely determine the hole number (n_{h}) of Pt in the Pt/Co/MgO. The moment values normalized by n_{h} are directly obtained from the sum rule formula without considering n_{h}^{35}. The changes in the induced magnetic moments with temperature are small (~15%) and comparable to the error range of the analysis as shown in Fig. 3b. This suggests that there is a weak correlation between the temperature dependences of the proximityinduced magnetic moments of the Pt layer and the DMI in the Pt/Co/MgO system^{11}.
Correlation between asymmetric orbital structure of the FM layer and the DMI
In this section, we study the correlation of DMI with various physical quantities associated with the magnetism of Co such as m_{s}, \({\boldsymbol{m}}_{\mathrm{o}}^\parallel\) and \({\boldsymbol{m}}_{\mathrm{o}}^ \bot\) and the intraatomic dipole moment m_{D}. As explained in the previous section, m_{s,eff} is the sum of m_{s} and m_{D}. The m_{s} and m_{D} values in terms of temperature were obtained from the relation \({\boldsymbol{m}}_{\mathrm{D}}\left( \theta \right) = {\boldsymbol{m}}_{\mathrm{D}}(0^\circ ) \cdot (1  3{\mathrm{cos}}^2\theta )\), thereby \({\boldsymbol{m}}_{{\mathrm{s}},{\mathrm{eff}}}\left( \theta \right) = {\boldsymbol{m}}_{\mathrm{s}} + {\boldsymbol{m}}_{\mathrm{D}}(0^\circ ) \cdot (1  3{\mathrm{cos}}^2\theta )\)^{28,34}.
Details about the sum rule calculation are explained in Supplementary Note 4. The XAS and XMCD of the film are measured at 100, 200 and 300 K. Two incident angles (θ=0° and 70° with respect to the film normal) were used to separately estimate \({\boldsymbol{m}}_{\mathrm{o}}^\parallel\) and \({\boldsymbol{m}}_{\mathrm{o}}^ \bot\) values using the relation \({\boldsymbol{m}}_{\mathrm{o}}\left( \theta \right) = {\boldsymbol{m}}_{\mathrm{o}}^ \bot {\mathrm{cos}}^2\theta + {\boldsymbol{m}}_{\mathrm{o}}^\parallel {\mathrm{sin}}^2\theta\)^{36}. Figure 4a, b are typical XAS and XMCD spectra at the Co L_{2,3} edges obtained at 0° and 300 K. The XMCD spectra show a clear temperature dependence of their intensity at both 0° and 70° as shown in Fig. 4c–f. In case of the m_{s}, it increases by 20% (from 0.87 μ_{B}/μ_{h} to 1.11 μ_{B}/n_{h}) as temperature decreases from 300 to 100 K (see Fig. 4g), which is consistent with the observed temperature dependence of M_{s}.
In addition to m_{s}, m_{D} shows a strong temperature dependence. The m_{D} reflects the anisotropy of f_{SD} distorted by the SOC or the crystalfield effect.^{28,29}. When the electron occupation becomes asymmetric, for instance, more electrons in the inplane orbitals than the outofplane orbitals, the situation gives rise to both nonzero m_{D} term and asymmetry in the charge distribution. As a result, asymmetry of the charge distribution naturally implies nonvanishing f_{SD} at transition metals' interfaces. As a result, the value of m_{D} determined from the sum rule analysis increases from 0.014 μ_{B}/n_{h} to 0.094 μ_{B}/n_{h} (Fig. 4g). In addition, the orbital anisotropy also increases as temperature decreases; \({\boldsymbol{m}}_o^ \bot\) increases from 0.058 μ_{B}/n_{h} to 0.080μ_{B}/n_{h}, whereas \({\boldsymbol{m}}_{\mathrm{o}}^\parallel\) slightly decreases from 0.044 μ_{B}/n_{h} to 0.039 μ_{B}/n_{h} (Fig. 4h). These results imply a correlation of DMI with m_{D} and orbital anisotropy. Since the variation of the perpendicular component of the m_{o} is also related to magnetocrystalline anisotropy (K_{U}) based on the Bruno theory^{37}, the correlation between DMI and K_{U} is also reasonable (see the Supplementary Note 5). Figure 5a shows \({\boldsymbol{m}}_{\mathrm{o}}^ \bot /{\boldsymbol{m}}_{\mathrm{o}}^\parallel\)(=[\({\boldsymbol{m}}_{\mathrm{o}}^ \bot (T)/{\boldsymbol{m}}_{\mathrm{o}}^\parallel (T)\)]/[\({\boldsymbol{m}}_{\mathrm{o}}^ \bot (300{\mathrm{K}})/{\boldsymbol{m}}_{\mathrm{o}}^\parallel (300{\mathrm{K}})\)]), and \({\boldsymbol{m}}_{\mathrm{D}}(T)/{\boldsymbol{m}}_{\mathrm{D}}(300{\mathrm{K}})\) plots as a function of the normalized D=D=(T)/D(300K) where T inside of parentheses is the measurement temperature. The ratio \({\boldsymbol{m}}_{\mathrm{o}}^ \bot /{\boldsymbol{m}}_{\mathrm{o}}^\parallel\) increases by 53% as D increases, and m_{D} also shows a clear correlation with the DMI; \({\boldsymbol{m}}_{\mathrm{D}}(100{\mathrm{K}})/{\boldsymbol{m}}_{\mathrm{D}}(300{\mathrm{K}})\)≈ 6.4. Because both orbital anisotropy and m_{D} are closely related to the orbital occupation with ISB^{28,37,38}, these results suggest that the temperature dependence of DMI is governed by the change in asymmetric electron occupation in orbitals in addition to spin magnetic moments as we discuss with the following theoretical studies. We also note that peak intensity of the XAS spectra reflects the hole number in 3d orbitals. We found small change in the absorption intensity when varying the temperature. Quantitatively, difference in the XAS intensity integral (I_{XAS}) between 300 and 100 K is about 4% \(\{ [I_{{\mathrm{XAS}}}\left( {300{\mathrm{K}}} \right)  I_{{\mathrm{XAS}}}\left( {100{\mathrm{K}}} \right)]/ I_{{\mathrm{XAS}}}\left( {300{\mathrm{K}}} \right) = 0.04\}\). Hence, this indicates that there is a small change in the hole number within the temperature range, reflecting temperature dependence of the charge distribution in orbitals. Nonetheless, the value is so small that it does not affect the trend in the respective quantities normalized by n_{h} from the sum rule calculation.
Theoretical consideration about the microscopic origin of the DMI
In order to support the insights obtained from our experimental study, we carry out two types of theoretical calculations: a tightbinding model calculation and ab initio calculation based on density function theory (DFT), and the main result is shown in Fig. 5b, c. The details of these two complementary theoretical studies can be found in Supplementary Notes 6 and 7.
For the tightbinding model, we extend the trimer model suggested by Kashid et al.^{10}, which contains two magnetic atoms coupled to a spin–orbit coupled nonmagnetic ion. Compared to Kashid’s trimer model, we add one more orbital (d_{ xz }) on the nonmagnetic site, enabling the computation of the orbital anisotropy (see details in Supplementary Note 6). In order to describe the temperature dependence of parameters in our trimer model, we assume the level broadening increases with the temperature. This broadening can be phenomenologically explained by magnetization fluctuations and the electron–phonon interaction given by atomic vibrations. As this model calculation is too simple, we do not aim to give a quantitative explanation of the experimental data but provide a qualitative understanding of the experimental result.
Figure 5b shows that the tightbinding model calculation reproduces qualitatively our experimental observations; both the DMI and \({\boldsymbol{m}}_{\mathrm{o}}^ \bot\) decrease with temperature, while the \({\boldsymbol{m}}_{\mathrm{o}}^\parallel\) is almost temperature independent. Note that the \({\boldsymbol{m}}_{\mathrm{o}}^ \bot\) and \({\boldsymbol{m}}_{\mathrm{o}}^\parallel\) cases are related to electron hopping with and without ISB, respectively (Supplementary Note 6). In addition, the ratio of the spin density distribution (\(f_{{\mathrm{SD}}}^ \bot\)/\(f_{{\mathrm{SD}}}^\parallel\)) between the inplane (xy) and outofplane (yz, xz) orbital states decreases as temperature increases as shown in the inset in Fig. 5b (In our tightbinding model, the spin distribution is defined as SD_{ n }=f_{n,↑}−f_{n,↓}, where f_{n,↑}(f_{n,↓}) is the occupation of spin up (down) state and n represents the orbital quantum state \(d_{xy}^A,d_{xy}^B,d_{xy}^C,d_{yz}^C,d_{xz}^C\).). This result implies that the spin distribution variation of the orbital states with ISB is key to change of the orbital moment and the DMI, which is in line with the following DFT result.
To examine the correlation between the DMI and the orbital anisotropy in realistic structures, we also perform ab initio calculations for Pt(111)/X ultrathin films, where X is a 3d transition metal (X=V, Cr, Mn, Fe, Co, Ni). Based on the experimental observation, the microscopic origin of the correlation between the DMI and the orbital anisotropy involves the impact of the temperature on 3dorbital magnetization and their electron filling. In this respect, it is instructive to vary the 3d transition metals on the Pt substrate and examine the general chemical trend. Details about this study are also discussed in Supplementary Note 7. Figure 5c shows the summary of the DFT calculation. Here changing the overlayer results in modification of the relative alignment between 3d and 5d orbitals and thereby in a modification of the charge distribution: more hybridization results in less asphericity of the charge distribution between the inplane and the outofplane, as reflected by the change in m_{D}. Our calculation results provide a physical insight on how the asymmetric charge distribution induces DMI. As we mentioned in the second section, DMI requires three ingredients: (i) SOC, (ii) magnetic exchange, and (iii) symmetry breaking. While the first two aspects are easily quantifiable, the latter is more difficult to apprehend. It has been reported that the larger the asymmetric spin distribution with symmetry breaking and SOC, the larger intradipole spin moment^{29}. Therefore, our experimental and theoretical studies propose a method to address the symmetry breaking term. Figure 5c explains this aspect explicitly. The Mn 3d orbitals and the Pt 5d orbitals provide large magnetic exchange and SOC, respectively. In addition, the dipole moment term becomes maximized with the hybridization between Mn 3d and Pt 5d orbitals. As a result, DMI is maximal. Furthermore, both the DMI and the orbital anisotropy follow the same trend in their signs: D^{tot} and \({\boldsymbol{m}}_{\mathrm{o}}^ \bot /{\boldsymbol{m}}_{\mathrm{o}}^\parallel\) at the Pt/V interface have negative sign, while those of other interfaces have positive sign. We also find the correlation between m_{s} and DMI as confirmed experimentally in this study and in ref. ^{32}. In contrast, our calculations do not reproduce the experimental correlation reported above between DMI and the induced moment. This may be because of the difference between the actual film stack (~3 monolayers of Co) and the simulated system (1 monolayer of Co). In fact, the total DMI is dominated by the contribution of the first Co monolayer at the Co/Pt interface, while the Heisenberg exchange, which is a source of the induced moment, is affected by the total number of Co overlayers. This is why our calculation, limited to one Co overlayer, well reproduces the correlation of DMI with spin and orbital moments, but not with the induced moment.
Now, the remaining question is how the orbital asphericity can give rise to DMI. At the interface, inplane orbitals of Co and outofplane orbitals of Pt are mixed through interatomic hybridization (in our tightbinding model: d_{ xy } of Co and d_{ yz } of Pt). In the presence of ISB, this hybridization results in a nonvanishing orbital angular momentum: the hopping trajectory of an electron produces an effective orbital angular momentum as illustrated in Fig. 6. Moreover, the large SOC on Pt mixes inplane and outofplane orbitals, which is accompanied by spin canting (in our tightbinding model: d_{ xy } and d_{ yz } orbitals on Pt site). In other words, the SOC on Pt converts the interfacial orbital angular momentum of hopping electrons into spin canting, resulting in a noncollinear magnetic texture. In spite of its simplicity, this picture intuitively explains how the orbital asphericity generates the spin canting. A similar idea has been reported in ref. ^{21}: the interfacial electric dipole induced by the asymmetric charge distribution results in chiral orbital angular momentum, and thereby spin canting via SOC. Although the latter approach is based on porbitals, it agrees with the intuitive picture based on dorbitals.
Discussion
Our experimental study on the temperature dependence of the DMI suggests that the interfacial DMI in FM/HM bilayers originates from Heisenberg exchange and the asymmetric charge distribution caused by the ISB, as evidenced by the orbital anisotropy and magnetic dipole moment (\({\boldsymbol{m}}_{\mathrm{o}}^ \bot /{\boldsymbol{m}}_{\mathrm{o}}^\parallel ,\) m_{D}). Our DFT simulation and tightbinding calculation provide a clear evidence of the close link between the DMI and orbital physics. Based on the theoretical discussions, the temperaturedependent m_{D} and m_{o} indicate that increase in the temperature promotes the phononinduced electron hopping between the outofplane and inplane orbitals, thereby resulting in a reduced asphericity (or reduced asymmetry) of f_{SD} over the dorbitals and thus quenching m_{D}.
In our experiment, however, the correlation between \({\boldsymbol{m}}_{\mathrm{o}}^ \bot /{\boldsymbol{m}}_{\mathrm{o}}^\parallel\) and the DMI is only semiquantitative, i.e. the temperaturedependent change in the DMI does not perfectly scale with the temperaturedependent change in \({\boldsymbol{m}}_{\mathrm{o}}^ \bot /{\boldsymbol{m}}_{\mathrm{o}}^\parallel\). This semiquantitative correlation between the DMI and m_{o} demands a more detailed discussion. In systems with ISB, \({\boldsymbol{m}}_{\mathrm{o}}^ \bot\) can be decomposed into ISBindependent part and ISBdependent part. Given that ISB is an essential ingredient for the DMI, there should be a direct correlation between the DMI and ISBdependent m_{o}, as evidenced by our tightbinding model calculation. However, \({\boldsymbol{m}}_{\mathrm{o}}^ \bot\) also has an ISBindependent part, which precludes a direct and quantitative correlation between the DMI and \({\boldsymbol{m}}_{\mathrm{o}}^ \bot\). This statement can be rephrased technically as the DMI involves only offdiagonal elements of the SOC operator^{10}, while m_{o} involves all of them. We note, however, that even with this uncertainty, the experimentally observed correlation between the DMI and m_{o} anisotropy for the Pt/Co/MgO structure is rather clear, implying that the ISBdependent m_{ o } would dominate over the ISBindependent one in this structure. Therefore, our findings based on both experimental and theoretical studies provide a link between orbital physics and spin–orbitrelated phenomena such as the DMI, which are essential for spin–orbitronic devices.
Method
Film preparation and device fabrication
Si/Ta (1.5)/Pt (2)/Co (0.5)/MgO (2)/HfO (5) (in nm) film with perpendicular magnetic anisotropy was deposited on an undoped Si substrate by direct current magnetron sputtering and the atomic layer deposition technique. A 5μmwide Hall crossstructure were fabricated using the photo lithography and the Ar ion milling. For the XMCD measurement, the same stack film was prepared.
Nucleation field measurement
Angulardependent coercivity of the Co/Pt Hall device was measured to estimate the H_{n} of the magnetic droplet at 300, 200, 150 and 100 K. The angle between magnetic field and the sample normal was varied from 0° to 89° rotating the electromagnet. At each angle, magnetic field was swept with in ±0.5 T to observe the coercivity. Details about this measurement are also discussed in ref. ^{24}.
XMCD measurement
Soft Xray: Soft Xray absorption spectra were measured using the total electron yield method with 96% circularly polarized incident Xrays at the BL25SU at SPring8. XMCDs at the Co L_{3} and L_{2} edges (in a range between 770 and 840 keV) were recorded in the helicityswitching mode with an applied magnetic field of 1.9 T. Homogeneity of the magnetic field was better than 99% for ɸ10 mm at the sample position. The incident light direction was inclined by 10° with respect to the magnetic field direction. Temperature was varied from 300 to 100 K using a continuous liquid He flowtype cryostat.
Hard Xray: XMCD experiments using hard Xrays were carried out at BL39XU of SPring8. A circularly polarized Xray beam with a high degree of circular polarization (>95%) was produced with a transmissiontype diamond Xray phase retarder of 1.4mm thickness. XAS of the film were observed at a 0.6 T magnetic field applied parallel to the Xray propagation direction of which an incident angle was 0° with respect to the surface normal. The Xray fluorescence yield mode was used to record the spectra. The Xray energy was scanned around the Pt L_{3} and L_{2} edges in a range between 11.5 and 3.5 keV, reversing the Xray photon helicity at 0.5 Hz. In this manner, two helicity dependent spectra I^{+} and I^{−} were recorded simultaneously. Here I^{+} and I^{−} denote the intensities when the incident photon momentum and the magnetization vectors are parallel and antiparallel, respectively. The XMCD spectrum, ΔI = I^{+}−I^{−}, is given by the difference of the two spectra. Detailed experimental setups for the soft and hard Xray MCD measurements are described elsewhere^{39,40}.
DFT calculation
To understand the behaviour of DMI in 3d/Pt(111) ultrathin films and its correlation with the orbital moment anisotropy (OMA) and magnetic dipole moment (T_{z}), we have performed DFT calculations in the local density approximation^{41} to the exchange correlation functional, using the full potential linearized augmented plane wave method in film geometry^{42} as implemented in the Jülich DFT code FLEUR^{43}. Both collinear and noncollinear magnetic states have been studied employing an asymmetric film consisting of six substrate layers of Pt covered by a pseudomorphic 3d monolayer on one side of the film at the distance optimized for the lowest collinear magnetic states. For the noncollinear calculations, we used p(1x1) unit cell applying the generalized Bloch theorem (http://www.flapw.de). The OMA is obtained at relaxed geometry as total energy difference for two different magnetization directions employing the force theorem (the principle axes point along hard and easy axis). We considered 512 and 1024 kpoints in the twodimensional Brillouin zone (2DBZ) for the scalar relativistic computation and the calculation with SOC treated within firstorder perturbation theory, respectively. Note that high computational accuracy is required since energy differences between different magnetic configurations are tiny (~meV) in the present case.
In order to investigate the DMI, first we selfconsistently calculate the total energy of homogeneous magnetic spin spirals employing the generalized Bloch theorem within the scalarrelativistic approach^{44}. We have considered the energy dispersion E(q) of planar spin spirals, which are the general solution of the Heisenberg Hamiltonian, i.e. states in which the magnetic moment of an atom site R_{ i } is given by M_{ i }=M[cos(q·R_{ i }), sin(q·R_{ i }), 0] where q is the wave vector propagation of the spin spiral. By imposing the Néel spin spirals along the high symmetry lines of 2DBZ, we can scan all possible magnetic configurations that can be described by a single qvector. So, varying the qvector with small steps along the paths connecting the high symmetry points, we find the welldefined magnetic phases of the hexagonal lattice: FM state at \({\bar{\mathrm \Gamma }}\)point (q=0), antiFM state at the \({\bar{\mathrm M}}\)point, and periodic 120° Néel state the \({\bar{\mathrm K}}\)point. When the energy E(q) along the high symmetry lines of 2DBZ is lower than any of the collinear magnetic phases studied previously, the system most likely adopts an incommensurate spinspiral magnetic ground state structure.
In a second step, we evaluate the DMI contribution from the energy dispersion of spin spirals by applying the SOC treated within firstorder perturbation theory combined with the spin spirals^{5,42}. Phenomenologically, the antisymmetric exchange interaction DMI has the typical form \(E_{{\mathrm{DM}}} = \mathop {\sum }\limits_{i,j} {\boldsymbol{D}}_{i,j} \cdot ({\boldsymbol{S}}_i \times {\boldsymbol{S}}_j)\), where D_{ i }_{,}_{ j } is the DM vector that determine the strength and sign of DMI and S_{ i } and S_{ j } are magnetic spin moments located on neighbouring atomic sites i and j, respectively. Considering the Néeltype outofplane configuration, the D_{ i }_{,}_{ j } vector should be oriented in plane and normal to the qvector. Note that DMI term must vanish for both configurations Néeltype inplane and Blochtype spin spirals due to symmetry arguments^{44}. According to our definition, the vector chirality reads \(\boldsymbol{C}= C\hat{\boldsymbol c} = {\boldsymbol{S}}_i \times {\boldsymbol{S}}_{i + 1}\), where the direction of the vector spin chirality \(\hat{\boldsymbol c}\) is considered as spin rotation axis. Thus the lefthanded (righthanded) spin spiral correspond to C = +1 (C = −1)^{45}.
Data availability
The data that support the findings of this study are available from the corresponding author upon reasonable request.
References
 1.
Dzyaloshinskii, I. E. Thermodynamic theory of weak ferromagnetism in antiferromagnetic substances. Sov. Phys. JETP 5, 1259–1272 (1957).
 2.
Moriya, T. Anisotropic superexchange interaction and weak ferromagnetism. Phys. Rev. 120, 91–98 (1960).
 3.
Mühlbauer, S. et al. Skyrmion lattice in a chiral magnet. Science 323, 915–919 (2009).
 4.
Yu, X. Z. et al. Realspace observation of a twodimensional skyrmion crystal. Nature 465, 901–904 (2010).
 5.
Heide, M., Bihlmayer, G. & Blügel, S. DzyaloshinskiiMoriya interaction accounting for the orientation of magnetic domains in ultrathin films: Fe/W(110). Phys. Rev. B 78, 140403 (2008). (R).
 6.
Thiaville, A., Rohart, S., Jué, É., Cros, V. & Fert, A. Dynamics of Dzyaloshinskii domain walls in ultrathin magnetic films. Europhys. Lett. 100, 57002 (2012).
 7.
Emori, S., Bauer, U., Ahn, S.M., Martinez, E. & Beach, G. S. D. Currentdriven dynamics of chiral ferromagnetic domain walls. Nat. Mater. 12, 611–616 (2013).
 8.
Fert, A., Cros, V. & Sampaio, J. Skyrmions on the track. Nat. Nanotech. 8, 152–156 (2013).
 9.
Bode, M. et al. Chiral magnetic order at surfaces driven by inversion asymmetry. Nature 447, 190–193 (2007).
 10.
Kashid, V. et al. DzyaloshinskiiMoriya interaction and chiral magnetism in 3d−5d zigzag chains: tightbinding model and ab initio calculations. Phys. Rev. B 90, 054412 (2014).
 11.
Ryu, K.S. et al. Chiral spin torque arising from proximityinduced magnetization. Nat. Commun. 5, 3910 (2014).
 12.
Yang, H., Thiaville, A., Rohart, S., Fert, A. & Chshiev, M. Anatomy of DzyaloshinskiiMoriya interaction at Co/Pt interfaces. Phys. Rev. Lett. 115, 267210 (2015).
 13.
Belabbes, A., Bihlmayer, G., Bechstedt, F., Blügel, S. & Manchon, A. Hund’s ruledriven DzyaloshinskiiMoriya interaction at 3d5d interfaces. Phys. Rev. Lett. 117, 247202 (2016).
 14.
Fert, A. & Levy, P. M. Role of anisotropic exchange interactions in determining the properties of spinglasses. Phys. Rev. Lett. 44, 1538 (1980).
 15.
Fert, A. & Levy, P. M. Anisotropy induced by nonmagnetic impurities in CuMn spinglass alloys. Phys. Rev. B 23, 4667 (1981).
 16.
Fert, A. Magnetic and transport properties of metallic multilayers. Mater. Sci. Forum 59, 439–480 (1990).
 17.
Kundu, A. & Zhang, S. DzyaloshinskiiMoriya interaction mediated by spinpolarized band with Rashba spinorbit coupling. Phys. Rev. B 92, 094434 (2015).
 18.
Kim, K.W. et al. Chirality from interfacial spinorbit coupling effects in magnetic bilayers. Phys. Rev. Lett. 111, 216601 (2013).
 19.
Kikuchi, T., Koretsune, T., Arita, R. & Tatara, G. DzyaloshinskiiMoriya interaction as a consequence of a Doppler shift due to spinorbitinduced intrinsic spin current. Phys. Rev. Lett. 116, 247201 (2016).
 20.
Yamamoto, K. et al. Interfacial DzyaloshinskiiMoriya interaction and orbital magnetic moments of metallic multilayer films. AIP Adv. 7, 056302 (2017).
 21.
Park, S. R. et al. Orbitalangularmomentum based origin of Rashbatype surface band splitting. Phys. Rev. Lett. 107, 156803 (2011).
 22.
Park, J.H., Kim, C. H., Lee, H.W. & Han, J. H. Orbital chirality and Rashba interaction in magnetic bands. Phys. Rev. B 87, 041301(R) (2013).
 23.
Boulle, O. et al. Room temperature chiral magnetic skyrmions in ultrathin magnetic nanostructures. Nat. Nanotech. 11, 449–454 (2016).
 24.
Kim, S. et al. Magnetic droplet nucleation with a homochiral Néel domain wall. Phys. Rev. B 95(22), 220402(R) (2017).
 25.
Giustino, F. Electronphonon interactions from first principles. Rev. Mod. Phys. 89, 015003 (2017).
 26.
Sakamaki, M. et al. Perpendicular magnetic anisotropy in a Pt/Co/Pt ultrathin film arising from a lattice distortion induced by ion irradiation. Phys. Rev. B 86, 024418 (2012).
 27.
Kim, M. et al. Contribution of individual interfaces in the MgO/Co/Pd trilayer to perpendicular magnetic anisotropy upon annealing. Appl. Phys. Lett. 106, 102404 (2015).
 28.
Wu, R. & Freeman, A. J. Limitation of the magneticcirculardichroism spin sum rule for transition metals and importance of the magnetic dipole term. Phys. Rev. L 73, 1994 (1994).
 29.
Šipr, O., Minár, J. & Ebert, H. Influence of spinorbit coupling on the magnetic dipole term T_{α}. Phys. Rev. B 94, 144406 (2016).
 30.
Pizzini, S. et al. Chiralityinduced asymmetric magnetic nucleation in Pt/Co/AlOx ultrathin microstructures. Phys. Rev. Lett. 113, 047203 (2014).
 31.
Je, S.G. et al. Asymmetric magnetic domainwall motion by the DzyaloshinskiiMoriya interaction. Phys. Rev. B 88, 214401 (2013).
 32.
Nembach, H. T., Shaw, J. M., Weiler, M., Jué, E. & Silva, T. J. Linear relation between Heisenberg exchange and interfacial DzyaloshinskiiMoriya interaction in metal films. Nat. Phys. 11, 825–829 (2015).
 33.
Carra, P., Thole, B. T., Altarelli, M. & Wang, X. Xray circular dichroism and local magnetic fields. Phys. Rev. Lett. 70, 694 (1993).
 34.
Stöhr, J. Exploring the microscopic origin of magnetic anisotropies with Xray magnetic circular dichroism (XMCD) spectroscopy. J. Magn. Magn. Mater. 200, 470–497 (1999).
 35.
Chen, C. T. et al. Experimental confirmation of the Xray magnetic circular dichroism sum rules for iron and cobalt. Phys. Rev. B 75, 152 (1995).
 36.
Stöhr, J. & König, H. Determination of spin and orbitalmoment anisotropies in transition metals by angledependent xray magnetic circular dichroism. Phys. Rev. B 75, 3748 (1995).
 37.
Bruno, P. Tightbinding approach to the orbital magnetic moment and magnetocrystalline anisotropy of transitionmetal monolayers. Phys. Rev. B 39, 1 (1989).
 38.
Oguchi, T. & Shishidou, T. Anisotropic property of magnetic dipole in bulk, surface, and overlayer systems. Phys. Rev. B 70, 024412 (2004).
 39.
Nakamura, K. et al. Development of a soft Xray magnetic circular circular dichroism spectrometer using a 1.9 T electromagnet at BL25SU of SPring8. J. Electron. Spectrosc. Relat. Phenom. 144, 1035–1038 (2005).
 40.
Suzuki, M. et al. Depth profile of spin and orbital magnetic moments in a subnanometer Pt film on Co. Phys. Rev. B 72, 054430 (2005).
 41.
Jung, S. W. et al. Currentinduced domain wall motion in a nanowire with perpendicular magnetic anisotropy. Appl. Phys. Lett. 92, 202508 (2008).
 42.
Perdew, J. P. & Zunger, A. Selfinteraction correction to densityfunctional approximations for manyelectron systems. Phys. Rev. B 23, 5048 (1981).
 43.
Wimmer, E., Krakauer, H., Weinert, M. & Freeman, A. J. Fullpotential selfconsistent linearizedaugmentedplanewave method for calculating the electronic structure of molecules and surfaces: O_{2} Molecule. Phys. Rev. B 24, 864 (1981).
 44.
Kurz, P., Förster, F., Nordström, L., Bihlmayer, G. & Blügel, S. Ab initio treatment of noncollinear magnets with the fullpotential linearized augmented plane wave method. Phys. Rev. B 69, 024415 (2004).
 45.
Heide, M., Bihlmayer, G. & Blügel, S. Describing Dzyaloshinskii–Moriya spirals from first principles. Phys. B Cond. Matter 404, 2678–2683 (2009).
Acknowledgements
We also thank H.W. Lee for fruitful discussion about the relation between the orbital magnetism and the DMI. This work was partly supported by JSPS KAKENHI Grant Numbers 15H05702, 26870300, 26870304, 26103002 and 25220604; JSPS Postdoctoral Fellowship program (Grant Number 2604316, P16314); Collaborative Research Program of the Institute for Chemical Research, Kyoto University; R & D project for ICT Key Technology of MEXT from the Japan Society for the Promotion of Science (JSPS) and the Cooperative Research Project Program of the Research Institute of Electrical Communication, Tohoku University. This work has also been performed with the approval of the SPring8 Program Advisory Committee (Proposal Nos. 2015A0117, 2015A0125). A.M. and A.B. acknowledge support from King Abdullah University of Science and Technology (KAUST) and fruitful discussiojns with S. Blügel and G. Bihlmayer. G.G., P.H.J. and K.J.L. also acknowledge support from the National Research Foundation of Korea (NRF2015M3D1A1070465, 2017R1A2B2006119). K.J.K. was supported by the National Research Foundation of Korea (NRF) grant funded by the Korea Government (MSIP) (Nos. 2017R1C1B2009686, NRF2016R1A5A1008184) and by the DGIST R&D Program of the Ministry of Science, ICT and Future Planning (17BT02). S.K. was supported by Priority Research Centers Program through the National Research Foundation of Korea (NRF) funded by the Ministry of Education (20090093818).
Author information
Affiliations
Contributions
S.K., K.U., K.J.K., T.M. and T.O. conceived and designed the study. S.K., K.U., T.K. and D.C. fabricated the device and performed the nucleation field measurement. S.K., D.H.K., P.H.J., T.M., K.J.K. and T.O. contributed to determine the DMIinduced effective field using the droplet model. S.K., M.S., Y.K., T.N. and K.J.K. designed and performed XMCD experiment and analysed the data. K.U. and K.Y characterizes the magnetic properties of films. A.B., A.M. and K.N. supported theoretical analyses with ab initio calculation. G.G. and K.J.L. supported the tightbinding model for the temperature dependence of the DMI and orbital magnetism. All authors discussed the results and wrote the manuscript.
Corresponding authors
Ethics declarations
Competing interests
The authors declare no competing interests.
Additional information
Publisher's note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.
Electronic supplementary material
Rights and permissions
Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/.
About this article
Cite this article
Kim, S., Ueda, K., Go, G. et al. Correlation of the Dzyaloshinskii–Moriya interaction with Heisenberg exchange and orbital asphericity. Nat Commun 9, 1648 (2018). https://doi.org/10.1038/s4146701804017x
Received:
Accepted:
Published:
Further reading

Ruderman–Kittel–Kasuya–Yosidatype interfacial Dzyaloshinskii–Moriya interaction in heavy metal/ferromagnet heterostructures
Nature Communications (2021)

Determination of the DzyaloshinskiiMoriya interaction using pattern recognition and machine learning
npj Computational Materials (2021)

The microscopic origin of DMI in magnetic bilayers and prediction of giant DMI in new bilayers
npj Computational Materials (2020)

Interfacial atomic layers for full emergence of interfacial Dzyaloshinskii–Moriya interaction
NPG Asia Materials (2020)

Longrange chiral exchange interaction in synthetic antiferromagnets
Nature Materials (2019)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.