Chirality from Interfacial Spin-Orbit Coupling Effects in Magnetic Bilayers

# Chirality from interfacial spin-orbit coupling effects in magnetic bilayers

## Abstract

As nanomagnetic devices scale to smaller sizes, spin-orbit coupling due to the broken structural inversion symmetry at interfaces becomes increasingly important. Here we study interfacial spin-orbit coupling effects in magnetic bilayers using a simple Rashba model. The spin-orbit coupling introduces chirality into the behavior of the electrons and through them into the energetics of the magnetization. In the derived form of the magnetization dynamics, all of the contributions that are linear in the spin-orbit coupling follow from this chirality, considerably simplifying the analysis. For these systems, an important consequence is a correlation between the Dzyaloshinskii-Moriya interaction and the spin-orbit torque. We use this correlation to analyze recent experiments.

###### pacs:

Magnetic bilayers that consist of an atomically thin ferromagnetic layer (such as Co) in contact with a nonmagnetic layer (such as Pt) with strong spin-orbit coupling have emerged as prototypical systems that exhibit very strong spin-orbit coupling effects. Strong spin-orbit coupling can enhance the efficiency of the electrical control of magnetization. A series of recent experiments Miron:2010 (); Miron:2011a (); Miron:2011b (); Liu:2012a () on magnetic bilayers report dramatic effects such as anomalously fast current-driven magnetic domain wall motion Miron:2011a () and reversible switching of single ferromagnetic layers by in-plane currents Miron:2011b (); Liu:2012a (). Strong spin-orbit coupling can introduce chirality into the magnetic ground state Bode:2007 (); Heinze:2011 (). This chirality is predicted Thiaville:2012 () to boost the electrical control of magnetic degrees of freedom even further as has been confirmed in two experiments Emori:2013 (); Ryu:2013 ().

Interfaces lack structural inversion symmetry, allowing interfacial spin-orbit coupling to play an expanded role. In magnetic bilayers, it generates various effects including the Dzyaloshinskii-Moriya (DM) interaction Dzyaloshinskii:1957 (); Moriya:1960 (); Fert:1990 () and the spin-orbit torque Obata:2008 (); Matos-Abiague:2009 (); Wang:2012 (); Kim:2012a (); Pesin:2012 (); vanderBijl:2012 (). Here, we examine a simple Rashba model of the interface region. We compute the equation of motion for a magnetization texture by integrating out the electron degrees of freedom. We report two main findings. The first is the correlation between the DM interaction and the spin-orbit torques. Spin-orbit torques arise from interfacial spin-orbit coupling but also from the bulk spin Hall effect, and the importance of each contribution is hotly debated Miron:2011b (); Liu:2012b (); Kim:2013 (); Haazen:2013 (); Freimuth:2013 (). The correlation we find opens a way to quantify the contribution from interfacial spin-orbit coupling by measuring the DM interaction, allowing one to disentangle the two contributions.

The second finding is that all linear effects of the interfacial spin-orbit coupling, including the DM interaction and the spin-orbit torque, can be captured through a simple mathematical construct, which we call a chiral derivative. The chiral derivative also shows in the equation of motion how each contribution that is linear in the spin-orbit coupling corresponds to a contribution that is present even in the absence of spin-orbit coupling. This correspondence provides a simple way to quantitatively predict and understand a wide variety of interfacial spin-orbit coupling effects allowed by symmetry vanderBijl:2012 (). In the last part of the Letter, we discuss briefly the extension to realistic situations, which go beyond the simple Rashba model.

Our analysis begins with the two-dimensional (2D) Rashba Hamiltonian

 H = Hkin+HR+Hexc+Himp (1) = p22me+αRℏσ⋅(p×^z)+Jσ⋅^m+Himp,

where is the 2D electron momentum in the plane, the vector of the Pauli matrices represents the electron spin, and . is a minimal model Obata:2008 (); Matos-Abiague:2009 (); Wang:2012 (); Kim:2012a (); Pesin:2012 (); vanderBijl:2012 () for electronic properties of the interface region between the ferromagnetic and nonmagnetic layers in magnetic bilayers, and captures the broken symmetries; breaks the time-reversal symmetry, and breaks the structural inversion symmetry. The last term describes the scattering by both spin-independent and quenched spin-dependent impurities. The latter part of contributes to the Gilbert damping and the nonadiabatic spin torque Kohno:2006 (); Duine:2007 ().

Here, we focus on effects of on the equation of motion for the magnetization up to order . These effects include the DM interaction and the spin-orbit torque. We neglect effects of order such as interface-induced magnetic anisotropy, contributions to Gilbert damping Garate:2009a (); Kim:2012b (), and to the nonadiabaticity parameter Garate:2009b (). We introduce the unitary transformation Aleiner:2011 (); Valin-Rodriguez:2011 ()

 (2)

where

 kR=2αRmeℏ2 (3)

and . rotates the electron spin around the direction by the angle , where . We also introduce the -dependent matrix , which achieves the same rotation of a classical vector such as . Upon the unitary transformation, one finds (Supplementary Material Supplement ())

 U†HU=Hkin+Jσ⋅^m′+H′imp+O(α2R), (4)

where

 ^m′=R−1^m (5)

and . We ignore the last term in Eq. (4) as higher order. is not identical to but they share the same impurity expectation values up to , which implies that has no effect to linear order on the Gilbert damping coefficient or the nonadiabaticity coefficient Kohno:2006 (); Duine:2007 (). Thus up to , may be identified with . Then the unitary transformation from to has eliminated at the expense of replacing by .

With this replacement, we compute the energy of the filled Fermi sea as a function of . Without , the energy can depend on only through spatial derivatives () since the energy cannot depend on the direction of when is homogeneous. For smoothly varying over length scales longer than the Fermi wavelength, the energy density may be expressed as the micromagnetic exchange interaction density , where is the interfacial exchange stiffness coefficient. Equation (4) implies that in the presence of , can be obtained simply by replacing with ; . One then uses the relation (Supplementary Information)

 ∂u^m′=∂u(R−1^m)=R−1~∂u^m, (6)

where the chiral derivative is defined by

 ~∂u^m=∂u^m+kR(^z×^u)×^m. (7)

Here is the unit vector along the direction . The second term in Eq. (7) arises from the derivative operator acting on the -dependent . in the presence of the interfacial spin-orbit coupling then becomes

 ε = A(∂x^m⋅∂x^m+∂y^m⋅∂y^m) +D[^y⋅(^m×∂x^m)−^x⋅(^m×∂y^m)]+O(α2R),

with

 D=2kRA. (9)

Note that the second term in Eq. (Chirality from Interfacial Spin-Orbit Coupling Effects in Magnetic Bilayers) is nothing but the interfacial DM interaction responsible for chiral magnetic order addressed recently Thiaville:2012 (); Emori:2013 (); Ryu:2013 (). A few remarks are in order. First, this derivation shows that the DM interaction is intimately related to the usual micromagnetic exchange interaction that exists even in the absence of interfacial spin-orbit coupling. This is the first example of the one-to-one correspondence and illustrates how the interfacial spin-orbit coupling generates a term in linear order from each term present in the absence of the spin-orbit coupling. Second, this mechanism for the DM interaction in an itinerant ferromagnet is similar to that of the Ruderman-Kittel-Kasuya-Yosida interaction in nonmagnetic systems acquiring the DM-like character Imamura:2004 (); Lounis:2012 () when conduction electrons are subject to interfacial spin-orbit coupling.

Next, we demonstrate the correlation between the DM interaction and the spin-orbit torque. Although the spin-orbit torque has already been derived from Eq. (1) in previous studies Obata:2008 (); Matos-Abiague:2009 (); Wang:2012 (); Kim:2012a (); Pesin:2012 (); vanderBijl:2012 (), we present below a derivation of the spin-orbit torque that shows the relationship between it and the DM interaction. Without , it is well known Ralph:2008 () that the total spin torque induced by an in-plane current density consists of the following two components,

 Tst=vs(^j⋅∇)^m−βvs^m×(^j⋅∇)^m, (10)

where the first and the second components are the adiabatic Tatara:2004 () and nonadiabatic Zhang:2004 (); Thiaville:2005 () spin toques, respectively. Here , , is the nonadiabaticity parameter Zhang:2004 (); Thiaville:2005 (), and the spin velocity , where is the polarization of the current, is the Landé factor, is the Bohr magneton, is the saturation magnetization, and () is the electron charge. In the presence of , Eqs. (4) and (6) imply that changes to

 Tst=vs(^j⋅~∇)^m−βvs^m×(^j⋅~∇)^m, (11)

where . One then obtains from Eq. (7)

 Tst = vs(^j⋅∇)^m−βvs^m×(^j⋅∇)^m + τfvs^m×(^j×^z)−τdvs^m×[^m×(^j×^z)].

The two terms in the second line are the two components of the spin-orbit torque. The first (second) component in the second line is called the fieldlike (dampinglike) spin-orbit torque and arises from the adiabatic (nonadiabatic) torque in the first line. This is the second example of the one-to-one correspondence. The chiral derivative fixes the coefficients of the two spin-orbit torque components to

 τf=kR, τd=βkR. (13)

When combined with Eq. (9), one finds

 τf=D/2A,τd=βD/2A. (14)

This correlation between the DM coefficient and the spin-orbit torque coefficients and is a key result of this work.

A recent experiment Emori:2013 () examined current-driven domain wall motion in the systems Pt/CoFe/MgO and Ta/CoFe/MgO and concluded that domain wall motion against (along) the electron flow in the former (latter) system is due to the product being positive (negative). According to Eqs. (9) and (13), should be of the same sign as regardless of since is positive by definition. Thus explaining the experimental results for Ta/CoFe/MgO within the interfacial spin-orbit coupling theory requires to be negative. Whereas can be negative, in most models and parameter ranges it is positive. We tentatively conclude that in Ta/CoFe/MgO Emori:2013 () has a different origin, the spin Hall effect being a plausible mechanism as argued in Ref. Emori:2013 (). For Pt/CoFe/MgO, on the other hand, the reported sign is consistent with the sign determined from Eqs. (9) and (13) if . The Pt-based structure in Ref. Ryu:2013 () also gave the same sign as Ref. Emori:2013 (). To investigate the origin of the spin-orbit torque in Pt/CoFe/MgO, we attempt a semiquantitative analysis. For the suggested values  mJ/m,  J/m in Ref. Emori:2013 (), Eq. (9) predicts  m. For , ,  Am, which are again from Ref. Emori:2013 (), Eq. (13) predicts the effective transverse field of the fieldlike spin-orbit torque and the effective longitudinal field of the dampinglike spin-orbit torque to have the magnitudes 1.3 mT and 0.52 mT, respectively, for  A/m. Here is the gyromagnetic ratio. The former value is in reasonable agreement with the measured value 2 mT considering uncertainty in the parameter values quoted above, whereas the latter value is about an order of magnitude smaller than the measured value 5 mT in Ref. Emori:2013 (). We thus conclude that the fieldlike spin-orbit torque of Pt/CoFe/MgO in Ref. Emori:2013 () is probably due to the interfacial spin-orbit coupling whereas the dampinglike spin-orbit torque is probably due to a different mechanism such as the bulk spin Hall effect. For the fieldlike spin-orbit torque of Pt/CoFe/MgO, the relative sign of with respect to is also consistent with the prediction of the interfacial spin-orbit coupling if is positive.

These two examples illustrate the idea that all linear effects of the interfacial spin-orbit coupling can be captured through the chiral derivative . To gain insight into its physical meaning, it is illustrative to take and examine the solution of , which forms a left-handed (for ) cycloidal spiral (Fig. 1), where precesses around the axis [ axis if ] as increases with the precession rate . This chiral precession gives the name, chiral derivative. Note that this precession is identical to the conduction electron spin precession caused by in nonmagnetic systems Datta:1990 (). Moreover when , also causes the same conduction electron spin precession as does. Thus effects of and become harmonious and the one-dimensional “half” of the 2D Hamiltonian (1) gets minimized when . Interestingly, the sum of the exchange energy and the DM interaction, namely , also gets minimized when . This is not a coincidence as this sum by definition should agree with the energy landscape of the Hamiltonian, which forces the value in Eq. (9).

One consequence of deriving the spin-orbit torque using the chiral derivative is that such a derivation shows that the spin-orbit torque is chiral when combined with the conventional spin torque just as the DM interaction is chiral when combined with the micromagnetic exchange interaction. For example, when is along the direction, the total torque in Eq. (11) vanishes even for finite if . As a side remark, the first and second terms in Eq. (11) are nothing but current-dependent corrections to the torques due to the total equilibrium energy density in Eq. (Chirality from Interfacial Spin-Orbit Coupling Effects in Magnetic Bilayers) and the Gilbert damping, respectively. This identification is a straightforward generalization of a previously reported counterpart; when is absent, the adiabatic and nonadiabatic spin torques in Eq. (10) are the current-dependent corrections to the torques due to the micromagnetic exchange interaction Xiao:2006 () and the Gilbert damping Garate:2009a ().

The anomalously fast current-driven domain wall motion demonstrated in Ref. Ryu:2013 () raises the possibility that chirally ordered magnetic structures Bode:2007 (); Heinze:2011 () such as topological Skyrmion lattices may be very efficiently controlled electrically. Such motion would be similar to the highly efficient electrically driven dynamics of a Skyrmion lattice in a system with bulk spin-orbit coupling such as the B20 structure Jonietz:2010 (). Flexible deformation of the Skyrmion lattice is proposed Iwasaki:2013 () as an important contribution to the high efficiency of current-driven dynamics in B20 structures. We expect Skyrmion lattices in magnetic bilayers to behave similarly because both systems are similarly frustrated. The chiral derivative is noncommutative, , so the energy landscape of the lattice structure is necessarily frustrated leading to the existence of many metastable structures with low excitation energies.

In a Skyrmion lattice, another linear effect of the interfacial spin-orbit coupling becomes important. Consider a Skyrmion lattice without interfacial spin-orbit coupling. The spatial variation of introduces a real space Berry phase Neubauer:2009 (), which can affect the electron transport through a Skyrmion lattice. It produces a fictitious magnetic field Volovik:1987 () , where is nothing but the Skyrmion number density Neubauer:2009 (). Here the upper and lower signs apply to majority (spin antiparallel to ) and minority (spin parallel to ) electrons, and thus this field is spin dependent. An experiment Heinze:2011 () on Fe/Ir bilayer reported the Skyrmion spacing of 1 nm. For a Skyrmion density of (1 nm), becomes of the order of T, which can significantly affect electron transport.

In the presence of interfacial spin-orbit coupling, the Berry-phase-derived field becomes chiral. Following the same procedure as above, one finds that is now given by , where , where

 bR=kR∇⋅^m/4π. (15)

We estimate the magnitude of for the Mn/W bilayer Bode:2007 (), for which left-handed cycloidal spiral with period 12 nm is reported. From the estimated value nm meV per Mn atom and nm meV per Mn atom, we find nm from Eq. (9), and becomes about 140 T. Thus for the left-handed cycloidal spiral, for which the Skyrmion density , the effective magnetic field is governed by this interfacial spin-orbit coupling contribution.

For completeness, we also discuss briefly the interfacial spin-orbit coupling contribution to the fictitious electric field , which is spin dependent and arises when varies in time. Without , it is known that , where the so-called adiabatic contribution Volovik:1987 (); Barnes:2007 (); Yang:2010 () is given by and the nonadiabatic contribution Duine:2008 (); Tserkovnyak:2008 () is given by . In the presence of , corrections arise. Recently some of us Kim:2012b () reported a correction term , and Ref. Tatara:2013 () reported another correction term , which are given by

 (eadiaR)u = −kR(^z×^u)⋅∂t^m, (16) (enonR)u = βkR(^z×^u)⋅(^m×∂t^m). (17)

Here we point out that the previously reported corrections can be derived almost trivially using the chiral derivative since and . This derivation also reveals the chiral nature of and . For the drift motion of chiral magnetic structures at 100 m/s, the parameter values of the Mn/W bilayer Bode:2007 () lead to the estimation that both and are of the order of V/m, which should be easily detectable.

So far we focused on magnetic bilayers. But these results should also be relevant for the high-mobility 2D electron gas formed at the interface between two different insulating oxide materials. One example is the LaAlO/SrTiO interface Ohtomo:2004 (), which has broken structural inversion symmetry Caviglia:2010 () and becomes magnetic Brinkman:2007 () under proper conditions.

Last, we briefly discuss how features of real systems might affect our conclusions. Two differences in realistic band structures, are that the energy-momentum dispersion is not parabolic and that there are multiple energy bands Park:2013 (). Another difference is that magnetic bilayers are not strictly 2D systems, unlike systems such as LaAlO/SrTiO. To test the effects of more realistic band structures, in the Supplementary Material Supplement (), we examine a tight-binding version of , which generates nonparabolic energy bands, and find that the relation (9) remains valid despite the nonparabolic dispersion. The two dimensionality is tested in a recent publication by some of us Haney:2013a (). There, we perform a three-dimensional Boltzmann calculation to address the interfacial spin-orbit coupling effect on the spin-orbit torque and obtain results, which are in qualitative agreement with those of the 2D Rashba model. On the basis of these observations, we expect that predictions of the simple Rashba model will survive at least qualitatively even in realistic situations and thus can serve as a good reference point for more quantitative future analysis.

To conclude, we examined effects of interfacial spin-orbit coupling using the Rashba model. We found that all linear effects of the interfacial spin-orbit coupling can be derived by replacing spatial derivatives with chiral derivatives. This allows these effects to be understood in terms of chiral generalizations of effects in the absence of spin-orbit coupling. One important consequence is a relationship between the DM interaction and the spin-orbit torque, such that measuring one should give a strong indication of the other.

###### Acknowledgements.
H.W. L. wishes to thank Ki-Seok Kim, F. Freimuth, S. Blügel, T. Silva, and P. Haney for critical comments and useful discussions. Financial support was provided by NRF Grants No. 2013R1A2A2A05006237 and No. 2011- 0030046 (H.W. L.) and No. 2013R1A2A2A01013188 (K. J. L.).

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