# Spin transfer torques generated by the anomalous Hall effect and anisotropic magnetoresistance.

###### Abstract

Spin-orbit coupling in ferromagnets gives rise to the anomalous Hall effect and the anisotropic magnetoresistance, both of which can be used to create spin-transfer torques in a similar manner as the spin Hall effect. In this paper we show how these effects can be used to reliably switch perpendicularly magnetized layers and to move domain walls. A drift-diffusion treatment of the anomalous Hall effect and the anisotropic magnetoresistance describes the spin currents that flow in directions perpendicular to the electric field. In systems with two ferromagnetic layers separated by a spacer layer, an in-plane electric field cause spin currents to be injected from one layer into the other, creating spin transfer torques. Unlike the related spin Hall effect in non-magnetic materials, the anomalous Hall effect and the anisotropic magnetoresistance allow control of the orientation of the injected spins, and hence torques, by changing the direction of the magnetization in the injecting layer. The torques on one layer show a rich angular dependence as a function of the orientation of the magnetization in the other layer. The control of the torques afforded by changing the orientation of the magnetization in a fixed layer makes it possible to reliably switch a perpendicularly magnetized free layer. Our calculated critical current densities for a representative CoFe/Cu/FePt structure show that the switching can be efficient for appropriate material choices. Similarly, control of the magnetization direction can drive domain wall motion, as shown for NiFe/Cu/NiFe structures.

## I Introduction

The use of spin-orbit coupling to generate spin-transfer torquesBerger:1984 (); Slonczewski:1996 (); Berger:1996 (); Stiles:2006 (); Ralph:2007 () raises the possibility of new types of devices and more efficient versions of existing devices. In general, the spin-orbit coupling in these studies has been provided by a non-magnetic heavy metal layer such as Pt. Here, we show that replacing this non-magnetic layer by a ferromagnetic layer and a thin spacer layer offers potential advantages in device design. In existing approaches, spin-orbit torquesAndo:2008 (); Liu:2011 () typically derive from the spin Hall effectDyakonov:1971 (); Hirsch:1999 (); Zhang:2000 () in the bulk of non-magnetic layers or from spin-orbit torques localized at the interface between such a layer and a ferromagnetic layer.Bychkov:1984 (); Edelstein:1990 (); Obata:2008 (); Manchon:2008 (); MatosAbiague:2009 (); Wang:2012 (); Kim:2012 (); Pesin:2012 (); Bijl:2012 () The resulting torques may lead to more efficient switching of memory elementsMiron:2011a (); Liu:2012a (); Garello:2013a (); Lee:2013 (); Lee:2014 () or domain wall motion.Miron:2011b (); Haazen:2013 (); Emori:2013 (); Ryu:2013 (); Yoshimura:2014 (); Seo:2012 (); Thiaville:2012 () Considerable experimentalKimJ:2013 (); Qiu:2013 (); Fan:2014 (); Liu:2014 (); Garello:2013 (); Qiu:2014 () and theoreticalHaney:2013a (); Haney:2013b (); Freimuth:2013 (); Freimuth:2014 (); Kurebayashi:2014 () work has been devoted to characterizing these torques so as to understand the details of their origin. However, device design possibilities based on heavy metal layers are somewhat limited by the fact that the form of the torques is determined by the geometry of the device, that is, the direction of the current flow and the interface normal. We show that replacing the non-magnetic heavy metal by a ferromagnetic layer and a thin spacer layer gives greater control over the form of the torque because it is controlled by the direction of the magnetization, which can be varied, rather than the geometry.

Historically, the earliest spintronic effects, discovered before the electron was known to have a spin, were the anisotropic magnetoresistance,Thomson:1857 (); McGuire:1975 () and the anomalous Hall effect.Kundt:1893 (); Pugh:1953 (); Karplus:1954 (); Sinitsyn:2008 (); Nagaosa:2010 () Both of these effects are caused by spin-orbit coupling, but because of the strong coupling between spin currents and charge currents in ferromagnets, these are typically discussed in terms of the resulting charge currents and voltages. Very recently, several groupsMiao:2013 (); Azevedo:2014 (); Wang:2014 (); Tsukahara:2014 (); Weiler:2014 () measured what they described as the inverse spin Hall effect in permalloy, a nickel-iron alloy. This result raises the point that a spin current will always accompany the charge current caused by the anomalous Hall effectZhang:2000 () and the spin current will vary with the angle between the magnetization and the charge current as in the anisotropic magnetoresistance. We show that both the anomalous Hall effect and anisotropic magnetoresistance can be exploited to generate spin currents and spin transfer torques in much the same way as the spin Hall effect.

The spin Hall effectDyakonov:1971 (); Hirsch:1999 (); Zhang:2000 () occurs in metals, particularly heavy metals with strong spin-orbit coupling. When an electric field is applied in a particular direction, a spin current flows in all directions perpendicular to the field with spins oriented perpendicularly to their flow. That is, for an electric field in the direction, there is a spin current in every direction perpendicular to the electric field with spins pointing in the direction. This spin current can be written in the form , where the second index of the tensor spin current refers to the real space direction of flow and the first index refers to the orientation of the spin that is flowing. is the electric field, is the spin Hall conductivity, and is the Levi-Civita symbol. Repeated indices (here ) are summed over (here summing over ). The spin current arises through either intrinsic mechanisms,Guo:2008 (); Tanaka:2008 () that is through the spin-orbit coupling in the band structure, or extrinsic mechanismsGradhand:2010 (); Lowitzer:2011 () through the spin-orbit coupling in the impurity scattering.

The same spin-orbit effects occur in ferromagnets but are complicated by the exchange potential that gives rise to spin split band structures and spin-dependent conductivities. One complication is that in a ferromagnet any spin that is transverse to the magnetization precesses rapidly, so any transverse spin accumulation or spin current dephases quickly due to this precession. Thus, it becomes a very good approximation to treat the spins in a ferromagnet as parallel or antiparallel to the magnetization. Then, the tensor spin current in a ferromagnet has spins pointing in the direction of the magnetization flowing in the direction, or . This feature plays a crucial role in the results below. It allows control of the direction of the spins injected into other layers due to spin-orbit effects simply by changing . Such control does not exist with the spin Hall effect where the direction the spins point when injected into another layers is , where is the interface normal direction.

A second complication is that majority and minority electrons see very different potentials so the spin-orbit scattering that gives rise to pure spin currents in non-magnets gives rise to a charge current as well as a spin current. This charge current is the current measured in the anomalous Hall effect, whose direction is given by . Therefore, the spin current excited by the anomalous Hall effect has spins pointing the direction flowing in the direction, that is

(1) |

The anomalous Hall conductivity, , describes the charge current due to the anomalous Hall effect, the associated polarization expresses the fact that this charge current is spin polarized.

The anisotropic magnetoresistanceThomson:1857 (); McGuire:1975 () is an additional consequence of spin-orbit coupling in ferromagnets. In this case, the conductivity of a ferromagnet is different if the magnetization is along the electric field direction or perpendicular to it. While not typically considered, the polarization of the conductivity will change in these two cases. Another consequence of the anisotropy in the conductivity occurs when the magnetization is at any angle other than collinear with or perpendicular to the electric field. For these other orientations of the magnetization, the charge current has an additional contribution, which flows in the direction of the magnetization. This current is frequently described as the planar Hall effect because for a thin film ferromagnet, an electric field gives rise to a Hall current (perpendicular to the electric field) when the magnetization is rotated in the plane of the film. The charge current direction due to the planar Hall effect is given by and again, the spins flowing with that current point the direction. Then, the anisotropic magnetoresistance gives rise to a spin current

(2) |

The conductivity, , describes the difference in the charge conductivity comparing cases with the magnetic field parallel and perpendicular to the electric field. The associated polarization expresses the fact that this change in the charge current is spin polarized. The spins both flow and point along the magnetization.

The spin currents associated with the anomalous Hall effect and the anisotropic magnetoresistance can replace those associated with the spin Hall effect as generators of torques with advantage of being able to control the orientation of the spins. Applying an electric field in the plane of a ferromagnetic layer generates charge and spin currents flowing perpendicular to it and into adjacent layers. Thus in a FM/NM/FM film, where FM and NM refer to ferromagnetic and non-magnetic layers respectively, an in-plane electric field generates spin currents flowing perpendicularly to the layers. These spin currents exert torques on the magnetizations in both layers. The advantage of this approach is the orientation of the flowing spins can be controlled by varying the directions of the magnetizations. The goal of this paper is to evaluate these spin transfer torques and show how they may be advantageous for some device applications. We develop the drift-diffusion equations in Sec. II and apply them to the case in which an electric current flows in the plane of a FM/NM/FM film. Details of the derivation are given in the Appendices. In Sec. III, we illustrate the angular dependence of the torque as both magnetizations are varied and then show how these torques can lead to effective magnetization switching and domain wall motion. We summarize our results in Sec. IV.

## Ii Derivation

In this section we present the drift diffusion equations in ferromagnets, accounting for the spin-orbit derived contributions to the transport. Since spin components transverse to the magnetization rapidly precess and dephase, they can be neglected. Then, the charge and spin currents are combinations of the majority and minority currents carried by spin- () electrons. In the presence of the Anomalous Hall (AH) effect and the anisotropic magnetoresistance (AMR) effect, the spin current densities are given by

(3) | |||||

(4) | |||||

where the (total) electric current density is . The longitudinal conductivity and conductivities due to the anomalous Hall effect and the anisotropic magnetoresistance effect are denoted as , , and , respectively, and their spin polarizations are denoted as , , and respectively. The spin-dependent electro-chemical potentials are denoted as . We define electro-chemical potential and spin accumulation as

(5) |

We emphasize that the ”(longitudinal) spin accumulation” used in Refs. Brataas:2001, ; Brataas:2006, ; Tserkovnyak:2005, , which will be used below, is defined as , which is twice the magnitude of . In terms of and , we find that

In terms of these current densities, the tensor spin current density is .

It is tempting to imagine that all three polarizations, , , and are the same, but there is no reason that they should be. The polarization of the longitudinal conductivity, is determined by the spin-dependent densities of states and particularly the spin-dependent scattering rates. It is typically between -1 and 1, with negative values for the rare cases in which the minority conductivity is higher than the majority. Values approach for half metals. Values greater than 1 or less than -1 would imply that one spin type move backwards. We are not aware of any such case.

The polarizations, , that of polarization of the anomalous Hall effect and , that of the anomalous Hall effect are not simply related to . For example, we can construct several contradictory arguments for the value of . If we imagine that the anomalous Hall effect were simply a deflection of all carriers in one direction and that these carriers then underwent the same spin-dependent scattering as the longitudinal current, we would guess that . If on the other hand, we imagine that the anomalous Hall effect originates from the spin Hall effect in which different spins are deflected in opposite directions and then each spin is subject to the same spin-dependent scattering, we might imagine that the majority and minority electrons flow in the opposite directions but are affected by the same spin dependent scattering as the conductivity. The reversed flow for the minority electrons essentially inverts the polarization . In fact, first principles calculationsprivatejulich () of the spin polarization of the anomalous Hall effect give results that vary widely and do not seem to agree with any simple model. Some of this variability can be understood from first principles calculationsTanaka:2008 () of the spin Hall effect, which show that the spin Hall conductivity depends sensitively on the Fermi level. The spin split-band structure of ferromagnets can be viewed in a simple approximation as just a shift in energies of the bands for one spin relative to the other, or equivalently the two spins see different Fermi energies. In this case, the minority and majority spins that are deflected in different directions are deflected by different potentials and will be deflected in different amounts. Therefore, part of the polarization of the anomalous Hall current comes from the energy dependence of the “underlying spin Hall effect.” Similarly, , the spin polarization of the anomalous Hall effect, is determined by the change in the spin-dependent scattering and as such gives no expectation to its value.

We are interested in the geometry, illustrated in Fig. 1(b), in which two ferromagnetic films are separated from each other by a thin non-magnetic layer that allows the magnetizations of the two layers to be oriented independently of each other. We assume that the interface normals lie in the -direction and the electric field is applied in the -direction. We ignore charge and spin currents that flow in the -direction because they do not couple to anything. In general, an electric field in the -direction would give rise to charge current flow in the z-direction, but the thin film geometry treated here prevents that. Except for the applied electric potential , only the -components of and are non-zero, i.e., and . The electric field adjusts itself so that no electric current flows in the -direction.

In a particular ferromagnetic layer, we can solve Eqs. (II) and (II) together with the diffusion equationValet:1993 ()

(8) |

where is the spin diffusion length. In Appendix A, we give the details the derivation of these solutions. Here we highlight some of the key steps. Forcing the charge current in the -direction to be zero dictates that the spin current in the z-direction have the form

(9) |

where the constants and are to be determined in Appendix A. The spin current is given in terms of two effective conductivities and . The former essentially gives the spin current that would result in a bulk material in response to a field in the -direction in which the transverse charge current were constrained to be zero. The latter gives the spin current in response to a spin accumulation, including the corrections due to the charge current itself being zero. The effective conductivities are

(10) | |||||

and

(11) | |||||

While the effective conductivities appear complicated, simplifies considerably in certain limits and gives simple illustrations of the main results of this paper. If the anisotropic magnetoresistance can be neglected, . Thus, there is a spin current whenever the magnetization has a component along the -direction, . This means that by tilting the magnetization out-of-plane, it is possible to get an out-of-plane component the spins flowing into the other layer, something not achievable with the spin Hall effect in non-magnetic materials. This feature is illustrated in Fig 1(b). The factor of arises from two contributions, the term proportional to is directly from the polarized current accompanying the anomalous Hall current. The term proportional to comes from the polarization of the “counter-flow” current that cancels the anomalous Hall current.

When the anomalous Hall effect can be neglected, . This expression is more complicated than that for the anomalous Hall effect above because the anisotropic magnetoresistance affects the conductivity in the -direction as captured by the last factor in this expression. As with the previous case, an out-of plane component of the magnetization gives an out-of-plane component to the spin current, . As with the previous case, the factor of appears from the polarized current due to the planar Hall effect and the counter-flow current that cancels the charge current of the planar Hall effect.

Computing the torques on both layers requires finding the spin accumulation and spin current throughout the structure. The spin current at the F/N interface is given in terms of the spin accumulation at the F/N interface and interface conductances.Brataas:2001 (); Brataas:2006 (); Tserkovnyak:2005 () The spin accumulation is found by applying appropriate boundary conditions to and as described in Appendix A. For a magnetic layer with interface (1) at and interface (2) at , we have

(12) | |||||

where is at the interface of the normal metal with ferromagnet . The spin current is then

(13) |

Here and are the dimensionless interface conductance and its spin polarization, respectively, which relates to the interface resistance via with k. The cross section area is denoted as . The real and imaginary parts of the mixing conductance are denoted as and , respectively. Note that the charge chemical potential does not appear because the fact that the charge current across the interface is zero allows us to relate the chemical potential difference to the longitudinal spin chemical potential difference and eliminate the former from the equation for the spin current.

The solutions of the spin accumulations in each ferromagnetic layer and the boundary conditions allow us to write the spin current in each ferromagnetic layer in terms of the just the spin accumulation in the non-magnetic layer

(14) | |||||

where is defined as

(15) |

and

(16) |

Similarly, the spin current at the F/N interface is given by

(17) |

In the structure in Fig 1, we separate the two ferromagnetic layers by a thin non-magnetic layer. We assume that this layer effectively breaks the exchange coupling between the two ferromagnetic layers. We also assume that it is still thinner than its mean free path and spin diffusion length, so that spin current injected at one interface transmits unchanged to the other interface. These assumptions imply that the spin current and spin accumulation in the spacer layer can be treated as constant. This condition means that , from which can be determined. Then, the spin torque acting on is obtained from

(18) |

where is the magnetic constant and, , , and are the gyromagnetic ratio, saturation magnetization, and volume of F, respectively.

Further progress requires taking these solutions for both ferromagnetic layers and solving for the spin accumulation in the non-magnetic layer. In general, the resulting torque can be written in the form

The superscripts on the effective conductivities refer to the damping-like, , and field-like, , components of the torque. However, a key point of this paper is that these damping-like and field-like torques are defined with respect to the orientation of the magnetization in the other layer, here , and not as for the spin Hall effect, the direction , where is the interface normal. See Fig. 1 for the comparison. The effective conductivities depend strongly on the directions of the magnetizations, and . In particular, they inherit the strong orientational dependence from . When the imaginary part of the mixing conductance can be neglected, the field-like torque vanishes. The spin torque acting on is obtained in a similar way. In Appendix B, we show how to compute the torques numerically for the general case and show some analytic forms for some special cases. In the next section, we present numerical results and investigate the consequences of these torques on switching and domain wall motion.

The derivation in this section is done using the drift-diffusion approach, as is typically used in the analysis of experiments using the spin Hall effect to generate spin transfer torques. This approximation does not capture the in-plane giant magnetoresistance effect because in the absence of spin orbit effects, there is no net spin current flowing from layer to layer. The simplest calculation to capture the current-in-plane giant magnetoresistance is based on the Boltzmann equation.Camley:1989 () When applied to the spin Hall effect and resulting torques, this approachHaney:2013a () yields quantitative but not qualitative differences in comparison with the drift diffusion approach. We expect the same to be true for the present calculations. It is also the case that the in-plane giant magnetoresistance, in the absence of spin-orbit coupling, does not lead to a spin transfer torque even though spin flow from each layer to the other.

## Iii Results

### iii.1 Angular dependence of torques

While the full solution of the torque for a general model is quite complicated, it can be qualitatively understood much more simply. Using the parameters in Table 1, we compute the torque for a variety of magnetization directions for two 5 nm thick NiFe layers and plot them in Fig. 2. For simplicity, we consider two cases, and , so we can show the effect of each separately. In the limit that both are much less than , the two contributions should add.

NiFe | CoFeB | FePt | units | ||||
---|---|---|---|---|---|---|---|

122 | 300 | 390 | nm | ||||

0.7 | 0.56 | 0.40 | |||||

0.5 | 0.5 | 0.5 | knm | ||||

0.7 | 0.83 | 0.83 | |||||

10.0 | 10.0 | 10.0 | nm | ||||

1.0 | 0.0 | 0.0 | nm | ||||

5.5 | 4.5 | 5.0 | nm | ||||

0.001 | 0.0 | 0.015 | |||||

0.06 | 0.0 | 0.0147 | |||||

5 | 0 | 1.5 | |||||

0.9 | 0 | -0.1 | |||||

0.86 | 0.456 | MA/m | |||||

0.0 | 0.569 | MA/m | |||||

0.23206 | 0.23206 | Mm/(A s) | |||||

0.01 | 0.01 |

Consider first the case in which there is only the anomalous Hall effect. We have assumed that the imaginary part of the mixing conductance is much less than the real part, so any field-like torque that is present is also much smaller than the damping-like contribution. The discussion in Sec. I that for the spin current due to the fixed layer with its magnetization in the direction, gives guidance for the approximate angular dependence of the torque. Since the spins in the spin current point in the direction, the damping-like torque varies like . When the magnetization is along the -axis, the torque has the same angular dependence as the spin Hall effect as seen in the heavy (red) curves of Fig. 2(e-j). That is, a damping-like torque with respect to the -axis. In this case, the out-of-plane torque, , (heavy red curve in Fig. 2(g)) is essentially zero when the magnetization is rotated in plane.

As the fixed layer magnetization is rotated out of plane (light (green) and dashed (blue) curves in Fig. 2(e-j)), the torque remains damping-like, , but it develops an out-pf-plane component, , even when the magnetization is rotated in plane, (light (green) and dashed (blue) curves in Fig. 2(g). This breaks the symmetry between , making it possible to reliably switch the magnetization, as discussed in the next section. However, as the polarizer magnetization is rotated toward the pole, the total size of the torque goes to zero because goes to zero when .

When the anomalous Hall effect is absent and the anisotropic magnetoresistance is present (Fig. 2(k-p)), the angular dependence is slightly more complicated. Recall from Sec. I that when the anomalous Hall effect is absent. If , the last factor can be neglected. In that case, the damping-like torque varies like . The spin current flows along the magnetization direction, so unless there is no spin current flow into the free layer. Thus, the torque is zero when the fixed layer magnetization is in-plane (heavy (red) curves in Fig. 2(k-p)). Otherwise, it has roughly a damping-like form with respect to the fixed layer magnetization. For the values of parameters we have assumed, there are deviations from the simple behavior expected when the spin-orbit effects are weak.

### iii.2 Magnetic Switching

One advantage of spin-orbit effects in ferromagnets, as compared to the spin Hall effect, is that the control over the direction of the incident spin current allows for the excitation of magnetization dynamics that cannot be excited by the spin Hall effect. An example of such dynamics is a switching of a perpendicularly magnetized free layer in the absence of an external field. In this section, we analytically compute the critical current for switching a perpendicular magnetization in F due to the anomalous Hall effect and anisotropic magnetoresistance effect in F. We verify the behavior by direct numerical simulation of the Landau-Lifshitz-Gilbert (LLG) equation.

For illustrative purposes, we simplify the generally complex dependence on relative angle of the magnetizations seen in Eq. (54) by treating a special case. We assume that F has neither the anomalous Hall effect nor the anisotropic magnetoresistance, i.e., , whereas F has both. The magnetization of F, , can move freely, whereas that of F, , points to an arbitrary fixed direction. The values of the parameters are taken from CoFeB free (F) layer and FePt pinned (F) layer, and summarized in Table 1.

The LLG equation for the magnetization in F, with the spin torque, Eq. (II), is

(20) |

where is the Gilbert damping constant, and is given by (see also Appendix B)

(21) |

We introduce the parameter (), which characterizes the dependence of the spin torque strength on the relative angle of the magnetizations,

(22) |

where or . We emphasize that , , , and depend on the direction of , according to their definition, Eqs. (10), (11), (15), (16), and (22). On the other hand, is independent of because the F layer does not show the anomalous Hall effect nor anisotropic magnetoresistance effect.

We assume that F is a perpendicular magnet with an anisotropy field given by , where is the perpendicular anisotropy field. In the absence of an electric field , the free layer magnetization is stable along the perpendicular axis. We assume that it starts along the -axis, i.e., . In the presence of the spin torque, the magnetization is destabilized, and starts to precess around the -axis. Assuming that and , we can linearize the LLG equation (see Appendix C) and determine the critical current

(23) |

Using Eq. (23), we can estimate the critical current for field-free switching of perpendicular layers. As an example, let us assume that F has the anomalous Hall effect only, i.e., and . In this case, is and Eq. (23) can be simplified to Eq. (62). We choose the pinned layer magnetization to be and take the parameter values given in Table 1. For 10 nm of FePt, which can be fixed in a partially out of plane configuration, as a polarizer and 1 nm of CoFeB, with perpendicular anisotropy, as a free layer, we find a critical current of A/m from Eq. (23). In Fig. 3, we show the magnetization dynamics obtained by numerically solving the LLG equation (20) for the electric current densities of (a) and (b) , respectively. The magnetization stays near the initial direction in (a), whereas it switches the direction to , showing the validity of Eq. (23).

Figure 4 shows the switching current as a function of the orientation of the fixed layer magnetization from Eq. (23), and verified by numerical simulation of the LLG equation. The three panels show switching due to the anomalous Hall effect and anisotropic magnetoresistance separately and combined. For the parameters chosen here, given in Table 1, the anomalous Hall effect is more efficient. The figure shows that the most efficient switching occurs when the polarizer magnetization is close to perpendicular (). The efficiency is determined by a competition between two effects. One effect is the efficiency of the spins at destabilizing the magnetization toward reversal. Spins injected perpendicular to the stable magnetization direction exert the greatest torque, but since they enhance precession only over half a period and suppress it over the other, they do not destabilize the magnetization. Electrons with moments antiparallel to the magnetization exert no torque, but when the magnetization fluctuates, they exert a torque that destabilizes the magnetization over the whole precession period. When the critical current is large enough, they overcome the damping and any fluctuations get magnified, leading to reversal. The counterbalancing effect is that when the pinned layer magnetization is collinear with the magnetization, it is also collinear with the film normal and the injected spin current goes to zero. So, the most efficient switching occurs with the pinned layer magnetization close to normal but not all the way there, maximizing the total perpendicular component of the injected spins. Switching due to the anomalous Hall effect and that due to anisotropic magnetoresistance depend differently on the azimuthal angle so for some orientations of the fixed layer magnetization, they compete, but for others they cooperate to reduce the critical current.

The critical current is minimized at an optimal direction of . Because of complex dependences of and on the magnetization direction, as shown in Eqs. (10) and (11), it is difficult to derive a formula of this optimal direction. However, for the F with the anomalous Hall effect only, we can derive the analytical formula of the optimum direction of ; see Appendix C.1. The result, for this set of parameters is , .

We can compare these results with the magnetization switching assisted by the spin Hall effect. In the spin Hall effect, spin current polarized along the direction is injected to the free layer. This situation is similar to a special case of switching by spin-orbit effects in ferromagnets in which the pinned layer magnetization is in the direction. It is useful to consider a generalized situation with the fixed layer magnetization in the -plane, with no anisotropic magnetoresistance. Then, simplifies and Eq. (23) has the factor in the denominator as seen in Eq. (62). This factor implies that diverges when points to the -direction ( and ) because the anomalous Hall effect does not induce spin current along the -direction when . The critical current also diverges when points to the -direction ( and ) because the spin-transfer torque never overcomes the damping torque as needed to enhance precession. This is the equivalent of switching by the spin Hall effect. While the spin-transfer torque can excite magnetization dynamics, when the fixed layer magnetization is along it does not overcome the damping and does not cause precession to become unstable.

It is possible to excite dynamics in perpendicularly magnetized samples with the spin Hall effect (or the anomalous Hall effect with ) as shown by Lee et al.Lee:2013 (). In fact, they demonstrate that it is possible to switch the magnetization. However, the switching they observe is not due to the spin transfer torque overcoming the damping, but rather is due to a large amplitude excitation due to the rapid onset of the current and hence torque. However, since nothing in the system breaks the symmetry between up and down, such switching is extremely sensitive to pulse duration and current amplitude. Lee et al.Lee:2013 () demonstrate such sensitivity in Fig. 1(b) of their paper. They derive an analytic form, Eq. (5), for the critical current that is independent of the damping parameter. This independence indicates that the switching mechanism is precessional, rather than due to overcoming damping. To switch the magnetization direction without such sensitivity, an in-plane magnetic field slightly tilted to the -direction has been used experimentally Liu:2012b (). The switching mechanism due to the anomalous Hall effect with a fixed layer with an out-of-plane component to the magnetization has the advantage of being largely independent of the current density or pulse duration for currents above the critical current. Another advantage is that the external field is unnecessary to switch the magnetization. It can also be significantly lower when the damping parameter is small, as is desirable in many magnetic devices.

### iii.3 Domain wall motion

The spin-orbit torques generated by ferromagnets can also be useful to displace in-plane magnetic domain walls, which we illustrate through two simple examples. We first consider the spin-valve illustrated in Fig. 5(a), with an in-plane domain wall in the free layer F1 and a uniform polarizer in the fixed layer F2. Due to the spin orbit effects in F2, a torque is generated on F1 that has the form : . To study the effect of this torque we consider a 1D modelSchryer:1974 () of a transverse wall profile with a domain wall width . The magnetization in the free layer, with the domain wall, is subject to a spin current from a fixed layer below. This spin current will cause a small tilting of the magnetization away from the long axis in all of the domains and will cause motion of the domain wall. We neglect the small tilting of the domains to get the following equations for the domain wall dynamics:

(24) | |||||

(25) |

Here is the domain wall position, the out-of-plane tilt angle and the shape anisotropy. At equilibrium in the absence of spin torques, is equal to zero and the domain wall lies in plane.

In the regime below Walker breakdown, the wall moves with a constant tilt angle and a steady velocity. Assuming the tilt is small, ,

(26) |

Since for typical values of the current density, the out-of-plane tilt is indeed small. The domain wall moves steadily only if the generated spin torque has a component along the -direction. This is not the case of the torque generated by pure spin Hall effect in a non-magnetic heavy metal, in which case the domain wall does not move.Khvalkovskiy:2013 () On the other hand, the spin-orbit torques generated by a ferromagnet can have components along both the and directions when the polarizer is tilted out-of-plane. If, as we did in the last section, we consider the case of the torque generated by just the anomalous Hall effect in F2, then

(27) | |||||

This behavior is shown in Fig. 5, in which we treat the motion for the case with the anomalous Hall effect and anisotropic magnetoresistance in both layers. However, since we assume the magnetization lies in the plane, the anisotropic magnetoresistance plays a negligible role. Fig. 5 shows a relatively large domain wall velocity for a modest charge current density of A/m and a very small out of plane tilt of less than a degree.

In the proposed spin-valve system, the current flowing in the ferromagnet through the domain wall will also give rise to the more familiar (intralayer) adiabatic and non-adiabatic spin-transfer torques on the domain wall, these can enhance or oppose the effect of the spin-orbit torques. In comparison, the domain wall velocity induced by these intralayer torques is :

(28) |

where is the current polarization and the proportionality factor between the non-adiabatic and adiabatic torques. The ratio of the velocities is

(29) |

where is a series of factors (see Eq. (27) of order one. In a typical material as NiFe, both the anomalous spin hall angle and the non-adiabatic parameter are close to 1 Miao:2013 (). However, the domain wall will be mainly driven by the anomalous Hall torque because the wall width is typically much bigger than the layer thickness for most systems.Metaxas:2013 ()

The other system we consider is the coupled domain wall system shown in Fig. 6(a). In the case of a fixed polarizer and a free layer , can exert a torque on . But if is no longer fixed, can also induce a torque on . If the magnetic configuration is well chosen, these reciprocal torques can add and enhance magnetization dynamics of the coupled system. This is the case for the double domain wall system with anti-parallel configuration shown in Fig. 6.

If both magnetic layers are unpinned, the domain walls in each layer are strongly coupled. Domain walls in wires with opposite in-plane magnetizations tilt out of plane significantly due to the dipolar interaction between them, as shown in Fig.6. In equilibrium, one domain wall has the out-of-plane tilt angle , and the other so that the out-of-plane component is in the same direction and the in-plane directions are opposite. This configuration is illustrated in the micromagnetic simulations in Fig. 6(b) where blue shows the out-of-plane component of the magnetization.micromagdetails () As the spacer thickness decreases, the dipolar fields on each domain wall increase, and the maximum out-of-plane tilt angle increases as shown in Fig. 6(b), reaching values close to 15 for spacer thicknesses typical of synthetic antiferromagnets.

In this configuration, the domain wall in polarizes the domain wall in (and reciprocally), and we can replace and respectively by and in Eq. (24). For small angle deviations from the equilibrium configuration, this immediately leads to

(30) |

Due to the particular symmetry of the anomalous Hall effect torques, the domain wall in acquires the same velocity: the motion of the coupled domain wall system is self-sustained. For small spacer thicknesses, the tilt angle is large, and velocities comparable to the single wall system with a uniform tilted fixed polarizer can be reached.

## Iv Summary

In this paper we develop a drift-diffusion approach to treat transport effects of spin-orbit coupling in ferromagnets. These include the anomalous Hall effect and the anisotropic magnetoresistance. In addition to the transverse charge currents that arise due to these effects, there are concomitant spin currents. These spin currents flow perpendicularly to the electric field, and so can be injected into layers perpendicular to the electrical current flow. When these other layers are ferromagnets with magnetizations that are not aligned with the original layer, they create spin transfer torques. Unlike the related spin Hall effect in non-magnetic materials, the ferromagnetic spin-orbit effects allow some control of the orientation of the injected spins. This control arises because the flowing spins in a ferromagnet are collinear with the magnetization. Changing the orientation of the magnetization changes the direction of the spins injected into other layers.

We compute the torques due to current flow for two ferromagnet layers separated by a thin non-magnetic layer. The control of the direction of the injected spins makes it is possible to switch perpendicularly magnetized layers more easily because of the possibility of an out-of-plane component of the torque. We also show that such torques make it possible to switch in-plane magnetized layers via propagation of transverse/vortex walls and can efficiently induce dynamics in coupled magnetic systems, e.g. coupled transverse domain walls.

###### Acknowledgements.

The authors thank Robert McMichael for useful discussions. JG acknowledges funding from the European Research Council Grant No. 259068.## Appendix A Solution of electro-chemical potential and spin accumulation

The and -components of Eq. (II) are explicitly given terms of and by

(31) |

(32) |

The continuity equation for electric current in steady state, , requires , where and are the integral constants whereas . The condition implies , whereas the other integral constant corresponds to a shift of the chemical potential, . Then, the electro-chemical potential is

(33) |

We assume that the spin accumulation obeys the diffusion equation, Eq. (8). The solution can be expressed as . Two integral constants, and , are determined as follows. Using Eq. (33), the -component of Eq. (II) is Eq. (9) and the spin current is . When the ferromagnet lies in the region , and the spin current densities at and are given by and , respectively, the integral constants, and are determined as

(34) |

(35) |

These give Eq. (12). In the geometry shown in Fig. 1, the spin current at the F/N interface is or , and it is zero at the outer boundaries. Using these boundary conditions, Eq. (13) can be rewritten as Eq. (14). Note that satisfies

(36) |

which becomes in the absence of the AMR effect, reproducing the diffusion equation in Ref. Valet:1993, .

## Appendix B Details of the Calculation

The spin current is calculated from Eqs. (14) and (17) by assuming the conservation of the spin current inside the N layer, i.e., . This condition leads to the following equations to determine the components of ;

(37) |

Here, the components of the matrix are given by

(38) | |||

(39) | |||

(40) | |||

(41) | |||

(42) | |||

(43) | |||

(44) | |||

(45) | |||

(46) |

The solution of can be obtained by calculating the inverse of . In Eq. (37), we added ”” and ”” after , , and to emphasize that these quantities depend explicitly on the magnetization direction through Eqs. (10), (11), (15), and (16). From we evaluate the spin currents, Eqs. (14) and (17). The LLG equations for and are, respectively, given by

(47) | |||