# Spin heat accumulation induced by tunneling from a ferromagnet

## Abstract

An electric current from a ferromagnet into a non-magnetic material can induce a spin-dependent electron temperature. Here it is shown that this spin heat accumulation, when created by tunneling from a ferromagnet, produces a non-negligible voltage signal that is comparable to that due to the coexisting electrical spin accumulation and can give a different Hanle spin precession signature. The effect is governed by the spin polarization of the Peltier coefficient of the tunnel contact, its Seebeck coefficient, and the spin heat resistance of the non-magnetic material, which is related to the electrical spin resistance by a spin-Wiedemann-Franz law. Moreover, spin heat injection is subject to a heat conductivity mismatch that is overcome if the tunnel interface has a sufficiently large resistance.

###### pacs:

72.25.Hg, 73.40.Gk, 72.20.Pa, 85.75.-dCreation and detection of spin information are at the heart of spintronics, the study and use of spin degrees of freedom Žutic *et al.* (2004). Electronic spin transport is described by a two-channel model where transport is separately considered for each spin () population Mott (1936); Fert and Campbell (1968); van Son *et al.* (1987). When a current is applied between a ferromagnetic contact and a non-magnetic material, it induces a spin accumulation described by a splitting of the electrochemical potentials of the two spin channels in the non-magnetic material Valet and Fert (1993); Jedema *et al.* (2002); Lou *et al.* (2006); Dash *et al.* (2009). Direct electrical detection of the spin accumulation is achieved via the Hanle effect, where a magnetic field induces spin precession and suppresses , giving a measurable voltage signal. Interestingly, spin current in ferromagnetic tunnel contacts can be created both by an electrical bias Tedrow and Meservey (1971); Meservey and Tedrow (1994) or by a thermal bias Le Breton *et al.* (2011); Jansen *et al.* (2012a). The latter approach of thermal spin injection is possible due to the spin dependence of thermoelectric properties in magnetic materials and nanodevices, which lead to interactions between spin and heat transport currently studied in the field of spin caloritronics Hatami *et al.* (2009); Bauer *et al.* (2012). This raises the question: do Hanle measurements only detect a difference in electrochemical potentials , as hitherto assumed, or also a difference in temperatures between the two spin channels?

In this work we address the creation and detection of a spin heat accumulation in a non-magnetic material via a ferromagnetic tunnel contact. It is considered here that tunneling transport is accompanied by a spin-dependent heat flow if the Peltier coefficient of the tunnel contact depends on spin, and that this produces a spin heat accumulation and an additional contribution to the voltage signal in a Hanle measurement. Spin heat accumulation is a concept previously studied theoretically within the context of metallic spin-valve structures Giazotto *et al.* (2007); Hatami *et al.* (2007); Heikkilä *et al.* (2010) and only very recently it has been observed as a spin-dependent heat conductance in metallic current-perpendicular-to-plane spin-valve nanopillars Dejene *et al.* (2013). Here, we provide an explicit evaluation for the spin heat accumulation at the tunnel interface between a ferromagnet and a non-magnetic material. Notably, we introduce the notion of an associated heat conductivity mismatch, similar to that for spin accumulation Schmidt *et al.* (2000); Rashba (2000); Fert and Jaffrès (2001); Takahashi and Maekawa (2003); Maassen *et al.* (2012), which limits the magnitude of spin heat accumulation and can be overcome with the tunnel interface. Most importantly, we show that the widely employed Hanle measurement to detect spin accumulation has another contribution from the spin heat accumulation that can be comparable in magnitude and has a line width set by the spin heat relaxation time. It cannot be neglected a priori and needs to be considered for a correct interpretation of experimental data.

We consider the case of a three-terminal geometry, where the same contact is used for driving an electrical current and measuring the voltage signal, as commonly used for spin injection into semiconductors Lou *et al.* (2006); Dash *et al.* (2009), although the basic physics also applies to other device geometries, such as the non-local one. Such a tunnel junction with a ferromagnetic electrode and a non-magnetic semiconductor electrode is depicted in Fig. 1. We describe each spin population in the non-magnetic material by a Fermi-Dirac distribution with spin-dependent temperatures and . This is strictly valid only when thermalization within each spin channel is sufficiently fast compared to energy exchange between the spin channels. In general, the distributions could be non-thermal and we should regard as effective temperatures Heikkilä *et al.* (2010); Dejene *et al.* (2013). For the ferromagnet we assume negligible spin and spin heat accumulations due to stronger spin-flip and inelastic scattering processes, so both spin channels are equilibrated at . We define an average electron temperature in the non-magnetic material, and a temperature difference across the contact. The charge tunnel currents and the *electronic* heat currents for each spin channel are then given by ?; ?; ?

(1) | |||||

(2) |

with the voltage across the junction and the *electronic* heat conductance of the tunnel barrier in units of [WmK]. Charge currents are in units of [Am], conductances in [] and heat currents in [Wm]. By definition, and correspond to electron flow and heat flow, respectively, from the ferromagnet to the semiconductor. Furthermore, the Onsager coefficient (thermoelectric conductance) is positive when the conductance below the Fermi energy is larger than that above it, so the spin-dependent Seebeck coefficient for hole-like transport ^{1}

First we proceed to find the spin current and the spin heat current injected into the non-magnetic material. The spin current , and the charge current , are obtained from Eq. (1)

(3) | |||||

(4) |

where we have defined the total conductances and , and their spin polarizations and .

The *total* heat current contains, in addition to the heat flow by electrons, a dominant contribution due to phonon transport across the tunnel contact. It is given by , where is the phonon heat conductance of the barrier (usually dominated by the interfaces Ju *et al.* (2005)), is the phonon temperature in the non-magnetic electrode, and we assume that in the ferromagnet phonons and electrons are fully equilibrated at . Phonon heat flow is not parameterized by the spin variable and does not contribute to the spin heat current across the barrier. Thus, the injected spin heat current is only due to the electrons and can be obtained from Eq. (2)

(5) | |||||

where we have defined the total electronic heat conductance of the tunnel contact , its polarization and used the relation .

Now we can evaluate the contribution of the spin heat accumulation to a Hanle measurement. Typically, a Hanle measurement involves the application of a constant electrical current at the tunnel junction while spin precession in a magnetic field perpendicular to the injected spins causes to go to zero. The decrease in depends on the product of the spin-relaxation time and the Larmor frequency , with the Landé g-factor, the Bohr magneton, and the reduced Planck constant. Importantly, spin precession would also cause to go to zero. This can be understood by considering a packet of hot spins polarized along and an equal amount of cold spins polarized along . A perpendicular field along causes a precession of each spin in the – plane and thereby a periodic oscillation of the temperature of the electrons with spin pointing along (or ) not (). If the precession frequency is much larger that the inverse of the time constant , associated with relaxation of the spin heat accumulation, then the time-average of goes to zero. Therefore, for such an electrically driven junction, and assuming that the spin-averaged temperatures of the electrodes remain constant, the corresponding Hanle signal can be obtained from Eq. (3)

(6) |

In addition to the well-known Hanle signal arising from the spin accumulation , there is a second up to now neglected contribution due to the spin heat accumulation . Note that the Hanle curve vs , due to suppression of , is Lorentzian Žutic *et al.* (2004) and has a width that is inversely proportional to the spin-relaxation time . Similarly, we expect that the suppression of yields a Lorentzian Hanle curve having a width that is inversely proportional to the spin heat relaxation time , such that . If is sufficiently different than , then the total Hanle signal will consist of two superimposed Hanle curves with different widths, as depicted in Fig. 2. We remark that the latter directly follows from the sum of two independent contributions to the voltage, conform Eq. (6). Interestingly, if a spin heat accumulation is present, interpreting the total Hanle signal purely in terms of a spin accumulation would lead to an underestimation of the spin-relaxation time .

Next, we evaluate the created spin accumulation and spin heat accumulation in the non-magnetic material. We consider a steady-state condition in which the spin current injected by tunneling is balanced by the spin current due to spin relaxation processes in the material Valet and Fert (1993), occurring over the spatial extent of . Similarly, the spin heat current injected by tunneling is balanced by the heat current between the two spin populations due to spin relaxation *and* inelastic scattering processes Heikkilä *et al.* (2010), occurring over the spatial extent of . To relate accumulations and injected currents we define a spin resistance and a spin heat resistance of the non-magnetic material

(7) | |||||

(8) |

where is a phenomenological parameter that describes the conversion of the spin current injected by tunneling, into a spin accumulation with a value of right at the tunnel interface, as before Jansen *et al.* (2012b). This definition does not require us to assume any specific profile of the spin accumulation in the non-magnetic material. If we do assume that the spin accumulation decays exponentially away from the tunnel interface with a spin-relaxation length Valet and Fert (1993), then the spin resistance per unit area is , where is the resistivity of the non-magnetic material Fert and Jaffrès (2001); Fert *et al.* (2007); Jaffrès *et al.* (2010). Similarly, the parameter is defined in terms of the injected spin heat current and the spin heat accumulation right at the tunnel interface.

Using the definition above for spin heat resistance we can obtain from Eqs. (5) and (8)

(9) | |||||

where is the tunnel resistance, and is the *electronic* thermal resistance of the tunnel barrier. The two terms within the square brackets represent the sources of spin-dependent heat flow. The first one is due to the spin heat current that accompanies the charge current across the tunnel contact, governed by the spin polarization of the Peltier coefficient Flipse *et al.* (2012). The second term is present when there is a temperature bias across the junction, driving a spin-dependent heat flow if the heat conductance of the tunnel barrier is spin dependent () Dejene *et al.* (2013). If transport through the tunnel barrier is elastic, the tunnel resistance and the electronic thermal resistance of the tunnel barrier are interrelated by the Wiedemann-Franz law Støvneng and Lipavský (1990)

(10) |

with the Lorentz number. This allows us to estimate the magnitude of and, together with Eqs. (3) and (9), to obtain an explicit evaluation of the spin heat accumulation in terms of the driving current . Furthermore, we can also obtain an explicit evaluation for the spin accumulation from Eqs. (3), (4) and (7). The resulting expressions are

(11) | |||||

(12) |

Note the similarity among the terms between curly brackets in Eqs. (11) and (12). The term in Eq. (11) corresponds to the known issue of conductivity mismatch Schmidt *et al.* (2000); Rashba (2000); Fert and Jaffrès (2001); Takahashi and Maekawa (2003); Maassen *et al.* (2012) which limits the magnitude of the spin accumulation due to back flow of the spins into the ferromagnet when . Remarkably, the term in Eq. (12) alludes to an analogous notion of a heat conductivity mismatch: if the heat resistance of the tunnel barrier is smaller than the spin heat resistance of the non-magnetic material, then the spin heat accumulation is reduced by back flow of the spin heat into the ferromagnet. In order to overcome the heat conductivity mismatch, one needs to fulfill the condition . Note that this is governed by the electronic heat resistance of the tunnel contact, since phonons cannot transport spin heat across the tunnel barrier. This concept is crucial to the creation of a large , which in recent experimental work was limited by highly transparent metallic contacts Dejene *et al.* (2013).

Finally, we evaluate the magnitude of the spin heat accumulation and its corresponding contribution to the Hanle signal. Both are fully described by Eqs. (6), (11) and (12). In the following, we avoid the in general lengthy solutions and proceed to make a few practical simplifications. First, we consider a junction that is driven *electrically*, not thermally, so that the spin accumulation is dominated by electrical spin injection. We therefore neglect the second term (due to Seebeck spin tunneling Le Breton *et al.* (2011)) and third term (due to a non-zero spin heat accumulation ) in Eq. (11), and retain only the first term proportional to . Note that the last term is expected to be smaller than 1 mV, and thus small compared to . Similarly, the dominant term in Eq. (12) for is the first term, proportional to (due to the spin-dependent Peltier effect). This is valid since ,
and is typically smaller than for reasonable values of and .

Still, there is one parameter with an unknown magnitude, the spin heat resistance of the non-magnetic material . It can be expressed as not ()

(13) |

This constitutes a type of spin-Wiedemann-Franz law, relating the electronic spin resistance to the spin heat resistance.
The parameter takes into account the inelastic scattering processes occurring within the non-magnetic material which increase the interspin heat exchange. These microscopic processes, described in Ref. Heikkilä *et al.*, 2010, correspond to electron-electron and electron-phonon interactions that cause relaxation of the spin heat accumulation and decrease . We remark that is related to the concept of a spin heat relaxation length in the regime of diffusive (heat) transport, with the corresponding diffusion constant being the same as that for charge transport since *electronic* heat transport is associated with electrons only.
In the case of an exponentially decaying spin (heat) accumulation it follows that , which in recent work Dejene *et al.* (2013) has been estimated to be for Cu at room temperature. Therefore, can indeed be of order one. In general we may expect , although the definition not () of does not preclude a value smaller than unity. At low temperatures inelastic scattering processes are reduced Heikkilä *et al.* (2010), so we expect elastic spin-flip scattering to be the dominant spin relaxation mechanism and . Using this result, we finally obtain for the Hanle signal

(14) |

where the first term is due to and the second term is due to .

The relative magnitude of the two contributions to the Hanle signal is governed by the ratio , by , and by the factor . The latter is unity for V/K, which, in the Sommerfeld approximation, is the maximum value with a non-negative entropy production, as required by the second law of thermodynamics Guttman *et al.* (1995). Previous work has shown that the Seebeck coefficient of a tunnel junction is indeed in the order of V/K Leavens and Aers (1987); Marschall and Majumdar (1993); Le Breton *et al.* (2011); Walter *et al.* (2011), and for the case of ferromagnetic electrodes is enhanced by magnons McCann and Fal’ko (2002, 2004). If , the Hanle signals due to and are then comparable in magnitude. Interestingly, both contributions always show the same sign, because there are only quadratic terms.

We conclude that the spin heat accumulation can make a significant contribution to the Hanle signal that cannot be neglected a priori. In principle, it can even be larger than the regular Hanle signal from the spin accumulation if , which can occur when since we have . However, the resulting enhancement of the Hanle signal is not sufficiently large to explain recent experiments in which Hanle signals that scale with the tunnel resistance and are many orders of magnitude larger than predicted by theory are observed
Tran *et al.* (2009); Li *et al.* (2011); Jeon *et al.* (2011); Uemura *et al.* (2012); Sharma *et al.* (2014); Txoperena *et al.* (2013); Han *et al.* (2013),
as recently reviewed Jansen (2012); Jansen *et al.* (2012b). It would require by several orders of magnitude. To estimate the magnitude of the spin heat accumulation we use Eq. (12) in the regime without heat conductivity mismatch (), and retain only the leading term, so we obtain
. For reasonable parameters at room temperature of , , and , a modest current density of would yield a spin heat accumulation of (for ).

The creation, manipulation, and detection of spin heat accumulation is a subject that is still in its infancy. The realization that it contributes to Hanle measurements, given the spin dependence of Peltier coefficients in magnetic tunnel contacts, makes it a non-negligible factor that needs to be taken into account in current studies of spin injection. It affects the magnitude and width of the Hanle curve and its variation with temperature, and is also expected to be present in (non)local spin-valve measurements. The analogy between spin and heat transport, here made explicit by the concept of a heat conductivity mismatch, opens opportunities to address fundamental questions about the relaxation of a spin heat accumulation. How do inelastic processes affect the magnitude of the parameter in the spin-Wiedemann-Franz law and the width of the Hanle curve, and how is this behavior modified under the presence of a strong spin-orbit coupling. And is it possible that , meaning that the spin heat relaxes slower than the spin accumulation?

###### Acknowledgements.

IJVM thanks F. K. Dejene for useful discussions. This work was financially supported by the Zernike Institute for Advanced Materials and the Netherlands Organisation for Scientific Research (NWO).## Appendix A Supplemental Material

## Appendix B Spin-Wiedemann-Franz law

Here we develop in more detail the concept of a spin-Wiedemann-Franz law used in the main text. First, we prove mathematically the aforementioned law for the case of a spin relaxation dominated by elastic spin-flip scattering. Next, we include inelastic relaxation processes and define the parameter . Finally, we show that for elastic spin-flip scattering a non-zero spin heat accumulation does not induce nor change the spin accumulation.

### b.1 Spin heat resistance and Wiedemann-Franz law

The standard way to compute the steady state value of the spin accumulation is to balance the net amount of spins injected per unit time , with the loss of spins due to spin relaxation in the non-magnetic material. The latter is governed by the spin resistance , for which is obtained if we assume that decays exponentially away from the tunnel interface with a spin-relaxation length Fert and Jaffrès (2001); Jaffrès *et al.* (2010); Fert *et al.* (2007). In a similar way we evaluate the spin heat resistance , which describes how effective a (non-equilibrium) spin heat accumulation is relaxed to zero in a non-magnetic material. Inelastic (electron-phonon and electron-electron) interactions are possible relaxation mechanisms. We shall include these later on, but we first discuss another mechanism, namely, elastic (or quasi-elastic) spin-flip scattering. The net effect is that it moves electrons above the Fermi energy from the hot spin reservoir to the cold spin reservoir, and simultaneously moves electrons below the Fermi energy in the opposite direction. This results in cooling of the hot spin reservoir and warming up of the colder spin reservoir, thus equalizing and . Note that there is no net flow of spin angular momentum if the spin-flip scattering rate is not dependent on energy (i.e., unlike a spin accumulation, a non-zero does not give rise to spin relaxation, even though spin-flip scattering is the relevant scattering process. See the last subsection for an explicit evaluation).

The energy flow between the two spin reservoirs in the non-magnetic material is denoted by the spin heat current per unit volume (in Wm). We also introduce , the volume spin heat conductance (in WmK) that connects the two spin reservoirs, such that

(15) |

The total energy flow is obtained by integrating over the full spatial extent of the spin heat accumulation, noting that according to heat diffusion, the spin heat accumulation is expected to decay exponentially with vertical distance from the injection interface. That is, , where is the spin heat relaxation length. In a steady state, the integrated has to be equal to the spin heat current that is injected through the tunnel interface. Thus

(16) | |||||

Comparing this to the relation that defines (Eq. (8) in the main text) we find that

(17) |

Below it is shown that if the spin heat accumulation relaxes via elastic or quasi-elastic spin-flip scattering (only), we have for

(18) |

Because in that case also , we finally obtain

(19) |

This is an important result, as it constitutes a type of spin-Wiedemann-Franz law, relating the electronic spin resistance to the spin heat resistance via the Lorentz number and the temperature.

The final task is to prove Eq. (18) for . We assume that the spin-flip scattering is predominantly elastic. The spectral (energy-resolved) spin heat current due to spin-flip scattering, , in units of WmeV, is then

(20) |

where is the energy with respect to the Fermi energy, is the Fermi-Dirac distribution function, is the density of states per spin in the non-magnetic material, and is the spin-flip time. The factor of 2 appears because each spin flip reduces the energy difference between the two spin reservoirs by two units of . Note that and the elastic spin-relaxation time are related by . If the density of states and the spin-flip time are not strongly dependent on energy, the spin heat current per unit volume is given by

(21) | |||||

The following relations are of use:

(22) | |||||

(23) | |||||

(24) |

where is the equilibrium distribution parameterized by and . Using these relations we have

(25) |

Inserting this into Eq. (21) gives

(26) |

The integral can be evaluated using the Sommerfeld expansion (see Eq. (3) of Hatami et al. Ref. Hatami *et al.*, 2009):

(27) | |||||

(28) |

We then obtain

(29) |

Next we use the generalized Einstein relation, , where is the carrier mobility, the diffusion constant, is the spin-integrated electron density, and is equivalent to (recall that the latter was defined per spin). Using the resistivity , , and , we obtain

(30) |

Comparing this to Eq. (15) gives

(31) |

just as it was already used in Eq. (18). Note that the spin heat current due to spin-flip scattering is proportional solely to . There is no contribution from the non-zero . This is a direct consequence of the assumption that the spin-flip time is not dependent on energy.

### b.2 Wiedemann-Franz law including inelastic relaxation

In the previous subsection we derived a Wiedemann-Franz type of law for spin resistance, under the assumption that the relaxation of the spin heat accumulation occurs exclusively via (quasi-) elastic spin-flip scattering. However, spin heat relaxation occurs also via inelastic scattering processes.

One inelastic process is electron-phonon (-) scattering. Phonons in the non-magnetic material cause an indirect energy flow from the hot spin reservoir to the cold spin reservoir, which can be understood as follows. In the presence of a non-zero , the temperature difference between electrons and phonons is spin dependent and given by and , respectively. As a result, the heat transfer to the phonons is spin dependent, which tends to equalize and . For the specific case where the phonon temperature is equal to the spin-averaged electron temperature , we have and .

Another process is inelastic electron-electron (-) scattering, which causes a direct energy flow between the two spin reservoirs in the non-magnetic material, which also tends to equalize and . Note that in the absence of spin-orbit scattering Heikkilä *et al.* (2010) the - interaction does not cause any additional relaxation of the spin accumulation , so its sole effect is to decrease .

Including relaxation via inelastic processes in the derivation of the spin-Wiedemann-Franz law has important effects. First, in Eq. (15) for the spin heat current induced by a non-zero , we must add the volume spin heat conductances and due to - and - interactions, respectively. Therefore,

(32) |

where we have kept to denote the term due to elastic spin-flip scattering, given by Eq. (31).

The second effect is that we can no longer set , as previously done in Eq. (17) for the spin heat resistance. Let us discuss this in more detail. In the regime of diffusive (heat) transport, we expect that , with the corresponding diffusion constant being the same as that for charge transport. This is a valid assumption since *electronic* heat transport is associated with electrons only. This is analogous to the case of electronic spin transport where the charge and spin diffusion coefficients coincide. On the other hand, the inelastic scattering processes contribute to the relaxation of the spin heat accumulation, and therefore affect . This spin heat relaxation time can be obtained by defining the inelastic contribution to it via

(33) |

such that, together with from Eq. (29), we have the total volume spin heat conductance

(34) |

where

(35) |

Note that . Using Eq. (29) we can now write

(36) |

For the case of , this reduces to . To parameterize the contribution of inelastic scattering to the interspin energy exchange we define a parameter as

(37) |

The spin heat resistance including inelastic relaxation processes is obtained after Eq. (17) as

(38) | |||||

where we have first inserted Eq. (36), then used Eq. (31) to eliminate and then used that . Finally, expressing the spin resistance due to elastic processes only in terms of the total spin resistance including inelastic processes, we finally obtain

(39) |

which is the spin-Wiedemann-Franz law as described in Eq. (13) of the main text.

### b.3 Spin relaxation with finite spin heat accumulation

For the sake of completeness, we evaluate the spin current due to elastic spin-flip scattering in the presence of a spin heat accumulation using the same approach as in the first subsection. It is demonstrated that a non-zero does not induce nor change the spin accumulation, provided that the spin-flip time (and the density of states around the Fermi level) are not dependent on energy in the relevant range of a few . The spectral spin current density per unit volume (in Am) is

(40) |

If and do not vary much around the Fermi energy, the integrated spin current in the presence of a non-zero and a non-zero is

(41) |

Using Eq. (25) as in the first subsection, this is rewritten as

(42) |

The second part of the integral, which contains vanishes (see Eq. (3) of Hatami et al. Ref. Hatami *et al.*, 2009). Thus, only a non-zero produces a net spin current and spin relaxation. Now, using

(43) |

and

(44) |

we obtain

(45) |

Assuming that , and using that in a steady state, the spatially integrated has to be equal to the spin current that is injected through the tunnel interface, we obtain

(46) | |||||

where is the spin resistance (in m), consistent with the definition of in Eq. (7) of the main text.

## Appendix C Hanle effect and Bloch equations

In this section we describe the dynamics of the spin accumulation and the spin heat accumulation due to the Hanle effect. A spin accumulation in a paramagnetic material implies that there is a net non-equilibrium magnetization or particle spin density . The particle spin density is linearly proportional to the spin accumulation if the latter is sufficiently small:

(47) | |||||

Similarly, if we denote the energy density by , then the energy spin density is proportional to the spin heat accumulation :

(48) | |||||

When a magnetic field is applied transverse to the initial spin direction (Hanle geometry), the electron magnetic moments precess at the Larmor frequency. In the next paragraph we first describe the resulting dynamics of the particle spin density using the Bloch equations, and then apply a similar analysis to the energy spin density to describe the dynamics of the spin heat accumulation.

The Bloch equations that describe the dynamics (precession and relaxation) of the particle spin density are:

(49) | |||||

(50) | |||||

(51) |

with the gyromagnetic ratio. For applied along the z-axis, and the boundary conditions and at , the solutions are:

(52) | |||||

(53) | |||||

(54) |

Thus, the precession of the magnetic moments in a transverse magnetic field causes the projection of the particle spin density onto the x and y axis to oscillate at the Larmor frequency, whereas spin relaxation causes an exponential decay. Since the particle spin density has a magnitude and a direction that varies in time, and the particle spin density is proportional to the spin accumulation, the latter also has a magnitude and direction that varies in time. Integrating over time gives a Lorentzian for the x-component of the particle spin density, and similarly for the x-component of the spin accumulation:

(55) |

The energy spin density describes the difference in the energy of electrons with spin pointing parallel () and antiparallel () to a given quantization axis. The precession of the electron magnetic moments in a transverse magnetic field causes the quantization axis to be time dependent, and hence the energy spin density also precesses at the Larmor frequency. To describe this, we introduce a similar set of Bloch equations, but now for the energy spin density, and taking into account that a different relaxation time should be used:

(56) | |||||

(57) | |||||

(58) |

Please note that the energy spin density can be defined even if the particle spin density is zero. For applied along the z-axis, and with similar boundary conditions ( and