Chiral magnets are a promising route towards dense magnetic storage technology due to their inherent nano-scale dimensions and energy efficient properties. Engineering chiral magnets requires atomic-level control of the magnetic exchange interactions, including the Dzyaloshinskii–Moriya interaction, which defines a rotational sense for the magnetization of two coupled magnetic moments. Here we show that the indirect conduction electron-mediated Dzyaloshinskii–Moriya interaction between two individual magnetic atoms on a metallic surface can be manipulated by changing the interatomic distance with the tip of a scanning tunnelling microscope. We quantify this interaction by comparing our measurements to a quantum magnetic model and ab-initio calculations yielding a map of the chiral ground states of pairs of atoms depending on the interatomic separation. The map enables tailoring the chirality of the magnetization in dilute atomic-scale magnets.
Chirality is a peculiar lack of symmetry, which is seeing an increasing importance in various fields of science from the structure of molecules1 to the magnetic properties of solids2. In the field of magnetism, chirality defines a rotational sense for the magnetization, which can rotate clockwise or counterclockwise along an axis of the magnetic object. Such chiral magnets have been recently shown to host many interesting properties that rely on this local rotation, or twisting, of the magnetization such as inducing new quantum information particles based on Majorana fermions3,4. So-called skyrmions5,6, a particular class of chiral magnetization structure, are attractive candidates for information technology as they are inherently nano-sized, and they respond more efficiently to spin-polarized currents7 as compared with conventional domain walls2,8,9. This energy-efficient aspect of chiral magnets, combined with their miniature dimensions, makes them technologically appealing as they can be integrated into current designs for high-density storage2,10. And yet, creating chiral magnets with a well-defined size or designed spin texture is a difficult task11,12 that has not been achieved yet in an atom-by-atom manner.
Central to the understanding of how chiral order emerges at the atomic scale is the Dzyaloshinskii–Moriya interaction (DMI)13,14, which is defined as EDMI=D ˙ (S1 × S2) (Fig. 1). The DMI is a fundamental ingredient responsible for twisting the magnetization of two coupled spins S1 and S2, as the overall energy can be reduced between the two spins by canting their relative orientation as dictated by the Dzyaloshinskii–Moriya (DM) vector D. Moriya proposed that the origin of this anisotropic magnetic exchange interaction can be derived by considering spin-orbit coupling within a superexchange model14. Later, Smith15 and Fert16 derived that DMI between S1 and S2 can also stem from an indirect exchange mechanism mediated by conduction electrons. Here, similar to the usual Ruderman–Kittel–Kasuya–Yosida (RKKY) interaction17, conduction electrons locally exchange-couple to the atomic spins becoming spin-polarized and thereby mediate an interaction. However, in addition, the electrons spin-orbit scatter at the non-magnetic host atoms (Fig. 1)15,16. This process leads to a long-range DMI between the atomic spins, where not only the amplitude, but also the orientation of the DM vector oscillates as a function of separation. The magnetization of the coupled pair of quantum spins with spin operators and can then be quantified by the following Hamiltonian:
It decomposes into an isotropic Heisenberg exchange interaction term (J), which takes into account the usual RKKY-like exchange that favours collinear orientations, a DMI term (D), which favours non-collinear spin orientations, a single spin magnetic anisotropy term (Ki), which locks each spin in a given orientation resulting from the interaction with the crystal field, and a Zeeman term, which considers the response of each spin to a magnetic field B as determined by the g-factors gi and the Bohr magneton μB. As the orientation of the DM vector in equation (1) dictates a sense of rotation of S2 compared with S1, the distance-dependent oscillation of D induced by the indirect exchange mechanism inherently contains the possibility to tune the chirality by the separation of the pair. Nevertheless, although the DMI interaction has been studied to a large extent for bulk5 or thin-film systems9,18, little is known experimentally about how the indirect conduction electron-mediated DMI emerges between individual atoms, as originally proposed by Smith15,16. Central to this understanding are methods that can interrogate exchange interactions19 with ultimate spatial resolution on surfaces17.
To this end, we probe the magnetic excitations of coupled pairs of single iron atoms on a Pt(111) surface by low-temperature inelastic scanning tunnelling spectroscopy (ISTS; see Methods section for details). The choice of Pt as a substrate is motivated by a large spin-orbit coupling20. It induces a considerable distance dependent, oscillatory DM interaction within the pair, which is of similar strength as the isotropic exchange over a wide range of iron atom distances in this system. We finally show how the chirality of the resulting highly non-collinear magnetization states of the pair can be tuned by tailoring the positions of the two atoms.
Spectroscopy of the uncoupled constituents outside of the pair
To minimize the effect of magnetic anisotropy, which is typically strong for atoms on surfaces20,21, we use a clean Fe atom and an Fe atom with two attached hydrogen atoms (FeH2), each with spin S=5/2, which exhibit a very weak magnetic anisotropy depending on their adsorption site, face-centered cubic (fcc) or hexagonal close-packed (hcp), on the substrate atomic lattice22,23. At zero magnetic field Bz, ISTS on FehcpH2 reveals a strong peak at zero bias characteristic for the Kondo effect23,24, whereas the bare Fe atom shows a symmetric step-like increase in conductance because of spin excitations of the magnetic ground state to the first excited state (Fig. 2a, grey curves). This zero-field splitting originates from the magnetic anisotropy. For Fehcp, we found K=0.08 meV, and for Fefcc, K=−0.19 meV (ref. 22). Owing to the small anisotropy in FehcpH2 (K=0.02 meV), at zero field all eigenstates are nearly degenerate23 at our base temperature and the Kondo impurity behaves paramagnetically25, making it extremely sensitive to the magnetic perturbations produced by J and D.
Distance-dependent splitting of the Kondo resonance
By changing the interatomic distance in artificially arranged pairs of atoms with the tip of the scanning tunnelling microscope (STM)26 (see Methods section and Supplementary Fig. 1 for details), we demonstrate that the magnetic excitations of each spin are modified by the indirect exchange interaction depending on the interaction strength (Fig. 2a,b). We create different pairs, by leaving the FehcpH2 stationary and moving the Fe atom to a chosen distance from the centre of the FehcpH2 impurity (Fig. 2b). ISTS on each individual atom of a fabricated pair (Fig. 2a), reveals a splitting of the Kondo resonance on FehcpH2 (ref. 27) with a correlated increase in energy of the spin excitation on Fe as compared with the isolated impurities (see grey spectra in the foreground), which indicates the magnetic coupling between the two impurities. To quantify this interaction to first approximation, the splitting of the Kondo resonance at zero magnetic field can be mimicked by the effect of an effective exchange field |Beff| (Fig. 2c; see Methods section for details)23. For this purpose, the Kondo spectra are fitted to a Kondo model25,28, which considers the weak coupling limit within perturbation theory (see Methods section for details). The resulting |Beff| reveals a strong distance-dependent oscillation illustrating the long-range nature of the magnetic coupling reminiscent of the RKKY interaction17,29. As the separation of the magnetic atoms in the pairs are too large for a significant contribution of direct or super-exchange, the behaviour in |Beff| strongly suggests that the observed coupling is due to the indirect substrate electron-mediated exchange mechanism.
Determination of Heisenberg and DM exchange
To disentangle the contributions of J and D to the observed indirect exchange interaction (Fig. 1)15, we monitor the simultaneous changes in both the Kondo resonance of FehcpH2 and the magnetic excitation of Fe as a function of an applied out-of-plane magnetic field (Bz). This is shown in Fig. 3a–d for a particular pair with d=8.31 Å. The corresponding data for pairs with other distances are described in Supplementary Note 1. With increasing Bz the Kondo resonance splits nearly linearly indicating that the impurity easily aligns to the magnetic field direction, with only a small deviation compared with an isolated FehcpH2 (ref. 23). However, Fehcp shows a Bz-dependent evolution, which largely deviates from the isolated impurity22. The magnetic excitation shows practically no shift up to Bz=6 T and does shift linearly to higher energies only for larger magnetic fields. For the isolated Fehcp atom, is required to overcome the easy-plane anisotropy and align the spin fully parallel to the magnetic field direction (that is, into the Sz=5/2 state). In the magnetic field-dependent map of the spin excitation of the isolated Fehcp atom22, this is manifested by a minimum in the excitation energy at Bz=3.0 T, which is induced by the level crossing of the Sz=5/2 and Sz=3/2 states, followed by a linear shift in the excitation at higher magnetic fields. The absence of this minimum for the Fehcp within the pair (Fig. 3d) signifies a strong magnetic coupling, which destroys the level crossing.
To understand how J and D separately affect the spectra, we simulate the measured ISTS of each atom considering the Hamiltonian equation (1) within the Kondo model (see Methods section for details)28 for different values of J and D and fixed values of K and g, which have been determined by fitting the isolated atoms (see Methods section for details). By considering the simplified superposition of the contributions of all substrate atoms to D shown in Fig. 1 we expect the out-of-plane component Dz as well as the in-plane component D||, which is parallel to the displacement vector between the two atoms, to be negligible for most of the pairs, whereas only the in-plane component D⊥ pointing perpendicular to the displacement vector survives due to the broken inversion symmetry induced by the surface. This is later confirmed by our first-principles calculations (see below). To reduce the number of parameters, we therefore set Dz=D||=0 and only consider the absolute value of D⊥. The latter restriction is furthermore justified as equation (1) does not contain any operators besides D that break the in-plane symmetry. Figure 3e,f exemplarily shows the simulated spectra for the d=8.31 Å pair that best fit the experimental ISTS (Fig. 3c,d) as determined by a variation of both, J and |D⊥|, whereas the same is shown in Fig. 3g,h but with the restriction of zero DMI (D⊥=0). Obviously, only when considering the combined effect of nonzero D and J, is it possible to excellently reproduce the trends in the experimental spectra for both FehcpH2 and Fehcp. In particular, the effect of nonzero D is to avoid the level crossings of the Fehcp spin states resulting in the experimentally observed absence of the above-mentioned minimum in the excitation energy. Moreover, the almost linear splitting of the FehcpH2 Kondo resonance, which behaves very similar to the splitting for the isolated impurity23, is nicely reproduced. The influence of the DMI on the magnetization is illustrated in Fig. 3i–l by the magnetic field-dependent expectation values of the spin in out-of-plane and parallel orientations (see Methods section for details). The most dramatic effect of D is the appearance of strong parallel components of the magnetization on both atoms in the pair (Fig. 3k,l). The parallel component is positive for FehcpH2 and negative for Fehcp at positive Bz, and vice versa for negative Bz, illustrating the creation of non-collinear, antiferromagnetic magnetization states. Moreover, the difference in the sign of the parallel components defines a rotational sense of the magnetization when going from FehcpH2 to Fehcp, demonstrating the chiral nature of the DMI.
Distance dependency of Dzyaloshinskii–Moriya exchange
It is interesting to investigate how the two indirect conduction electron-mediated exchange components D and J vary as a function of distance. It has been shown that the sign and amplitude of J is distance dependent, as determined by the electronic structure of the atom/substrate complex17. However, it is not a priori clear if the twisting and the chirality induced by D oscillates in a similar way30,31. To this extent, we vary the separation d between the atoms in the pair and perform a similar measurement and analysis as shown in Fig. 3 in order to extract J and |D⊥| for all pairs (Supplementary Note 1) within an errorbar whose estimation we explain in Supplementary Note 2. The resulting distance dependence shown in Fig. 4a,b reveals a damped oscillation in J between antiferromagnetic (J<0) and ferromagnetic (J>0) coupling, which reflects the well-known behaviour of indirect conduction electron-mediated Heisenberg exchange17. More importantly, we see that also |D⊥| shows a strong distance dependence, and long-range oscillations with an apparently smaller wavelength as compared with J, which we discuss below. This oscillatory behaviour of |D⊥| further substantiates that the origin for the observed DMI is indirect conduction electron-mediated exchange as proposed by Smith15. As we have shown for Co/Pt(111), this indirect exchange interaction between single atoms is intricately related to the electronic structure17, and first-principles calculations have shown reasonable agreement with the experimental values of J. To understand the distance-dependent evolution of J and D, we therefore employed first-principles calculations based on density functional theory as implemented in the full-potential Korringa–Kohn–Rostoker Green function (KKR) method (see Methods section for details)32, which includes spin-orbit coupling.
The theoretical results are summarized and compared with the experimental values in Fig. 4a–c, where we compare the experimentally extracted values of J and |D⊥| to calculations for Fehcp-Fehcp pairs using a mapping to a classical Heisenberg model (see Methods section for details). The values of J shown in Fig. 4a are obtained after taking the trace of the tensor of exchange interactions for the two adatoms. We note that the variation between the different diagonal terms of the tensor is extremely small, justifying the use of an isotropic J in our model Hamiltonian. Moreover, although in principle also biquadratic exchange interaction can contribute to the Hamiltonian, this contribution turns out to be negligible when the distance between the magnetic atoms is large (see Methods section for details). By comparison of the length of D to the in-plane component and to D⊥ (Fig. 4b,c), we see theoretically that the D⊥ component is the dominant term compared with the other components of D for most of the pairs. Only at distances d<9 Å, small but significant values of Dz lead to a deviation between D* and D⊥ (Supplementary Note 3). This justifies the simplified determination of negligible components of D via the construction illustrated in Fig. 1 and the restriction to D⊥ used in the simulations of the experimental spectra. Most importantly, the calculated Dplane quantitatively reproduces the experimentally determined values of |D⊥|, in particular the apparently smaller wavelength of the oscillation of |D⊥| as compared with that of J. As the experimental determination is not sensitive to the sign of D⊥, the oscillations are more clearly revealed by the calculated values of D⊥ shown in Fig. 4c. These oscillations indeed show sign changes on a much shorter length scale as the oscillations in J. This is qualitatively expected already from the simple model where the interactions are mediated by a quasi-free electron gas15. Here, the long-range form of J is given by sin(2kFd), whereas that of D is given by sin(kF[RA+RB+d]), where RA and RB are the distances of the two atoms A and B of the pair to the substrate atom mediating the DMI (Fig. 1). As RA+RB+d≥2d, the DMI is expected to oscillate on a smaller length scale as the Heisenberg exchange. However, it should be noted that the realistic band structure of the substrate, which yields highly anisotropic energy contours in k-space, results in a more complex behaviour than expected from these simple models17.
The oscillation of the sign of the dominating DM component D⊥ illustrated in Fig. 4c directly implies that the orientation of D changes as a function of the separation of the pair, namely between pointing to the left or to the right looking along the displacement vector between the two atoms. As the DMI favours a particular rotational sense of the magnetization in the pair which depends on the orientation of D (equation (1)), the oscillations have a direct consequence on the preferred chirality of the magnetization in the pair. This is visualized in Fig. 4d–f, where we show the parallel components of the expectation values of the spins of three antiferromagnetic pairs with positive (d,f) and negative (e) D⊥. At positive Bz, the sign in D⊥ leads to a negative/positive parallel component on FehcpH2/Fehcp for D⊥>0 and vice versa for D⊥<0. Taking into account the z-components of the expectation values of the spins, this implies a clockwise or counterclockwise rotation of the magnetization, respectively, when going from FehcpH2 to Fehcp, as indicated by the magnetization vectors in the insets of Fig. 4d–f (see Supplementary Movie 1 for details).
The oscillation in the indirect conduction electron-mediated DM interaction proposed by Smith in 1976 (ref. 15), which we experimentally verify here, consequently enables tailored chirality of the magnetization in pairs of atoms by tuning the interatomic distance. More specifically, by changing the interatomic distance, the strength of the DMI can be of the same magnitude or even larger than that of the isotropic exchange interaction, which drives collinear order. The measured and calculated interaction maps (Fig. 4), combined with small magnetic anisotropy energies23 enables a class of bottom-up magnets with tunable chirality, for example, of a two-dimensional nature, such as magnetic skyrmions9, down to one-dimensional systems, such as spin spirals33.
Experimental equipment, tip and sample preparation
All experiments were performed with an STM in an ultrahigh vacuum facility at 0.3 K (ref. 34). A magnetic field Bz of up to 12 T can be applied perpendicular to the sample surface. Topography images were obtained in constant-current mode with stabilization current Is and voltage Vs applied to the sample. The ISTS were obtained by using a lock-in technique to record the differential conductance while ramping the bias voltage (VS) after the feedback loop was switched off, by adding an AC modulation voltage Vmod (given in rms) to the bias voltage.
We used a clean tungsten tip and a tungsten tip that was initially coated with nominally 50 monolayers of chromium before inserting it into the STM as described in ref. 34. For the ISTS shown here, both tips were afterwards prepared by voltage-pulsing and dipping into the platinum surface until almost featureless spectra on platinum and close to symmetric spectra on the magnetic atoms were achieved.
The Pt(111) single crystal was cleaned by alternating Ar+ sputtering (high voltage=2 kV) and annealing (≈740 °C) cycles of decreasing duration. An oxygen annealing procedure has been performed for 1 h at ≈660 °C and an O2 pressure in the chamber of 2 × 10−6 mbar. The final flash was carried out at ≈1000 °C for 1 min and a background pressure of 5.5 × 10−10 mbar.
Finally, Fe was deposited onto the clean Pt(111) surface. To obtain single atoms on the surface, the crystal was cooled to <10 K during deposition. This resulted in a statistical distribution of Fe atoms adsorbed to the fcc (Fefcc) or hcp (Fehcp) hollow sites of the Pt(111) surface, where the adsorption site can be identified by the characteristic ISTS spectra22. In addition, we recorded an atomic manipulation image in Supplementary Fig. 1a by recording a constant current image with an adatom partly bound to the tip35. This allows us to exactly determine the lattice of the Pt(111) surface and to align the direction of close packed Pt surface atoms parallel to the fast scan direction.
After long-term exposure of the sample to H2 from the residual gas of the ultrahigh vacuum chamber, some of the Fe atoms form Fe–H complexes with one or two attached H atoms. Using ISTS, the complex with two attached H atoms where the Fe is sitting on the hcp site (FehcpH2) can be identified by a characteristic Kondo peak in ISTS spectra23. Although clean Fe can be laterally manipulated between the two different hollow adsorption sites with typical manipulation parameters (Vs=2 mV, Is=40–60 nA), it is not possible to manipulate FehcpH2 without de-attaching at least one H atom. Therefore, for the creation of the different pairs investigated here, FehcpH2 was kept stationary and Fe was moved to different positions. The Pt lattice determined by the atomic manipulation image together with the spectroscopic information from ISTS enables unambiguous determination of the absolute positions of the atoms in the pairs with respect to the Pt lattice underneath. Examples for two pairs with different distances, angles and adsorption sites are given in Supplementary Fig. 1b,c.
Model for simulations of conductance spectra and magnetization curves
To extract the values for the Heisenberg coupling J and the DMI D from our experiments, we used a third-order perturbation theory model25,28 to fit and simulate our spectroscopic data. The Hamiltonian for a number n of impurities in this model consists of a Zeeman and an anisotropy term and looks like this:
with gi as the gyromagnetic factors, μB the Bohr magneton, B the applied magnetic field, the vector of spin matrices of the impurity and Ki the uniaxial anisotropy constant.
An additional coupling Hamiltonian considers the isotropic Heisenberg and the anisotropic DMI between all pairs of atoms. The interaction Hamiltonian then looks like the following:
We calculate conductance spectra using a perturbative model where we take into account the scattering matrices up to the third-order using the following Kondo-like interaction matrix between the localized spin system and the electrons, which tunnel between tip and sample:
Here, represent the initial and final wave functions of the probed spin, are the electron states in sample or tip, respectively, are the standard Pauli spin matrices and U the Coulomb scattering term, which was negligibly small for most calculations. In addition, spin–spin interactions of electrons originating and ending in the substrate were accounted for any spin, not only the one the tip is placed above. This matrix transition element results then in
Here, ℑρS is the dimensionless coupling strength between the sample electrons and the localized spin with ℑ as the coupling energy and ρS the density of states in the sample close to the Fermi energy.
For all simulations we used an electron bandwidth ω0=20 mV and an effective temperature Teff=0.6 K, which best describes the effective linewidth of the excitations22. The anisotropies as well as the gyromagnetic factors of the three unperturbed impurities (Fehcp, Fefcc, FehcpH2) are known from earlier work22,23 and additionally have been extracted here by fitting spectroscopic data on individual impurities to the above model. The resulting parameters of the gyromagnetic factors g and uniaxial anisotropies are , , , , , . The coupling strengths ℑρS, which also resulted from these fits, were ℑρS=−0.12 for FehcpH2, ℑρS=−0.02 for Fehcp and ℑρS=−0.002 for Fefcc. Thus, we are left with the coupling constants J and D, which we determine by calculating the conductance spectra for numerous settings and find the best match to the experimental data. To account for small drifts in the junction during measurements, we additionally allowed a small background slope and offset in dI/dV.
For the determination of the effective exchange field |Beff|, which mimics the splitting of the Kondo resonance, we fit the conductance spectra from the above model for a single magnetic atom, that is, without the interaction terms, to the data of the coupled Kondo atom, by adjusting B keeping g=2.
The same model has been used to calculate the spin-expectation values in out-of-plane , parallel and perpendicular orientations (see assignment of directions in Fig. 1) as a function of B. These expectation values are proportional to the components of the magnetization of the impurities. Please note that, for the Kondo impurity FehcpH2, this is strictly only fully accurate as long as B is large enough to quench the Kondo screening23.
The electronic and magnetic properties of the investigated dimers were obtained theoretically utilizing the full-potential KKR method32,36 that is based on density functional theory. Spin-orbit coupling was included self-consistently as it is an essential ingredient in the physics of the DMI.
In this type of investigation, the Pt(111) surface is first computed and then an embedding scheme based on the Green functions is employed to deposit the Fe adatoms on the substrate. The surface is simulated with a slab of 22 Pt layers augmented by two vacuum regions using the experimental lattice parameter of Pt (3.92 Å). To describe the adatoms, a real space cluster surrounding the adatoms is constructed. Pt is a 5d transition element that is initially non-magnetic but thanks to its high magnetic polarizability, it easily can develop a magnetic moment in the vicinity of Fe (ref. 22). This is also the case for the dimers. Thus, around each adatom, there is manifestation of a large induced spin-polarization cloud. Our previous calculations showed that, in order to reasonably describe the magnetic properties of an Fe adatom, the polarization of ∼60 Pt atoms neighbouring the impurity need to be taken into account22. Thus, for the dimers, twice this number of Pt atoms has to be included in our simulations. For the distances between the adatoms considered experimentally, the total magnetic moment of the dimers and substrate, including the spin and orbital components in the ferromagnetic state, reaches a large value of the order of ∼10μB, 95% of which originates from the spin component. As soon as a hydrogen atom is attached to one of the adatoms, the total magnetic moment decreases by ∼0.8μB. These results motivated our choice of attributing a spin of 5/2 for each Fe adatom in our model simulations.
Once the ferromagnetic state is obtained for all the considered dimers, a mapping procedure to a classical Heisenberg model is performed in order to extract the tensor of magnetic exchange interactions JT (refs 37, 38). In this case, the Heisenberg Hamiltonian without the magnetic anisotropy energy and Zeeman term can be written as
where α=(x, y, z) and G12 being the Green function connecting the atoms 1 and 2. δVα represents the change of the adatom’s potential upon infinitesimal rotation along the direction α. The prefactor S(S+1) takes care of the normalization followed in the model-based calculations presented in the main text. The trace of this tensor divided by 3 gives rise to the isotropic Heisenberg exchange interactions, whereas the antisymmetric part leads to the DMIs37,38. As can be seen from the previous equation, the presence of the Green function explains the oscillatory behaviour of J and D with respect to the mutual distance between the adatoms. Basically, the elements of the tensor JT are described by electrons propagating from atom 1 to atom 2 and back while experiencing scattering at the magnetic part of both potentials.
Although, in principle, the whole tensor can be utilized to build a generalized Heisenberg Hamiltonian, we analysed its properties in order to reduce the quantities to be fitted experimentally to the most relevant ones and ended up with equation (1). Higher-order terms can be in principle added to the Hamiltonian in equation (1), for instance the so-called biquadratic term which is proportional to . However, and as verified in our simulations, such a term is dramatically small for the distances considered experimentally. This is expected as the biquadratic contribution involves terms containing four Green functions that would describe the double propagation of electrons and their scattering at both adatoms when compared with the regular bilinear term J. Thus, the distance-dependent decay of the biquadratic interactions is expected to be stronger than the one characterizing J.
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A.A.K., M.S., J.W. and R.W. acknowledge funding from the SFB668 and the GrK1286 of the DFG. A.A.K. acknowledges funding from the Emmy Noether Program from the DFG, and the Dutch funding agencies FOM, which is part of NWO, and NWO (VIDI program). M.T. acknowledges support from the SFB 767. M.B., M.S.D. and S.L. acknowledge discussions and support from S. Blügel and funding from the HGF-YIG Programme FunSiLab (VH-NG-717) and the DFG project (LO 1659 5-1).
The authors declare no competing financial interests.
Supplementary Figure 1-6, Supplementary Table 1 and Supplementary Notes 1-3 (PDF 1731 kb)
The movie shows the magnetic field (Bz given at the bottom of each panel) dependent evolution of the calculated expectation values 〈Ŝz〉 (vertical axis) and 〈Ŝ‖〉 (horizontal axis) of FehcpH2 (left red line) and Fehcp (right red line) for three pairs of different separation d and signs of the perpendicular component of the Dzyaloshinskii-Moriya vector (D⊥) given on the top. It illustrates the resulting clockwise (left and right panels) and counterclockwise (middle panel) rotation of the magnetization. (MOV 1141 kb)
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Khajetoorians, A., Steinbrecher, M., Ternes, M. et al. Tailoring the chiral magnetic interaction between two individual atoms. Nat Commun 7, 10620 (2016) doi:10.1038/ncomms10620
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