Temperature-dependent charge transport in the compensated ferrimagnet Mn{}_{1.5}V{}_{0.5}FeAl from first principles

Temperature-dependent charge transport in the compensated ferrimagnet MnVFeAl from first principles

R. Stinshoff Max-Planck-Institut für Chemische Physik fester Stoffe, 01187 Dresden, Germany    S. Wimmer    H. Ebert Ludwig-Maximilians-Universität, Dept. Chemie, Butenandtstr. 11, 81377 München, Germany    G. H. Fecher    C. Felser    S. Chadov Max-Planck-Institut für Chemische Physik fester Stoffe, 01187 Dresden, Germany stanislav.chadov@cpfs.mpg.de
Abstract

We present an ab-initio study of the temperature-dependent longitudinal and anomalous Hall resistivities in the compensated collinear ferrimagnet MnVFeAl. Its transport properties are calculated using the general fully relativistic Kubo–Bastin formalism and their temperature dependency is accounted for magnetic and structural disorder. Both scattering sources, together with the residual chemical disorder, were treated equally provided by the CPA (Coherent Potential Approximation) SPR-KKR (Spin-Polarized Relativistic Korringa-Kohn-Rostoker) method. All calculated properties showed good agreement with a recent experimental results, providing useful specific information on the chemical and magnetic arrangement as well as on the influence of disorder. Finally, we demonstrated that the anomalous Hall effect in such compensated systems occurs regardless of the vanishing net spin moment.

compensated ferrimagnets, conductivity, anomalous Hall effect, disorder
pacs:
75.50.Gg, 72.80.Ng, 85.30.Fg

Magnetically compensated systems provide an attractive base for the next generation of spintronic devices MacDonald and Tsoi (2011). Their investigation is motivated by potential applications in various technological fields, such as new types of RAM, detectors, microscopic tips, etc, in which the interest is focused on an alternative manipulation of spins, absence of stray fields and higher operating frequencies. Magnetically compensated systems have different order parameters than ferromagnets, such as staggered magnetization Barthem et al. (2013); Wadley et al. (2016) or magnetic chirality van der Bijl et al. (2013); Watanabe et al. (2016); Singh et al. (2016), which can be manipulated and detected by either magnetic fields or pulsed electric currents. However, the absence of net magnetization does not exclude the possibility that such materials will exhibit the anomalous Hall effect (AHE) Kübler and Felser (2014), Kerr effect Feng et al. (2015) or high spin-polarization Chadov et al. (2013); Wollmann et al. (2015a); Chadov et al. (2015). For example, in case of the planar noncollinear antiferromagnets (e.g., MnIr) AHE has been predicted Chen et al. (2014) for the case when the mirror symmetry is broken. By considering magnetic compensation in the cubic ferrimagnets, it is important to note that, both typical cubic structures with Fm  m or 3m space groups correspond to I4/mmm or I  m2 magnetic space groups, respectively. Both cases belong to the magnetic Laue group 4/mmm Kleiner (1966); Seemann et al. (2015) which leads to the following shape of the conductivity tensor:

(1)

where is the anomalous Hall component. Obviously, will have a non-vanishing amplitude if there is a difference between the spin-up and -down projections of the electronic structure, which can be fulfilled if the magnetic moment of one atom type is compensated by the antiparallel moments from the other atom types. It is particularly easy to realize such systems using cubic Heusler alloys since most of them obey the Slater–Pauling rule Slater (1936); Pauling (1938), suggesting that compensated ferrimagnets can be found among compounds having 24 electron formula units. Some compensated Heusler ferrimagnets have been already reported, such as MnCoGa Li et al. (2013). Ferrimagnetic compensation can also be induced in the tetragonal structures Wollmann et al. (2015b), e.g., in the case of MnPtGa Nayak et al. (2015); however, the deviation from the Slater–Pauling rule does not allow for a clear recipe for the exact compensating stoichiometry.

The first experimental evidence of non-zero AHE in compensated cubic ferrimagnets was given recently Stinshoff et al. (2017a, b) for the Heusler compound MnVFeAl. Additional calculations Stinshoff et al. (2017b) have shown that this system is half-metallic in agreement with the Slater-Pauling rule, indicating that the observed AHE is due to the aforementioned strong asymmetry of the spin-channels. Here, we investigate this scenario by first-principles calculations on the system MnVFeAl and verify that the experimental non-zero AHE is an intrinsic property of the compensated ferrimagnets, rather than a consequence of the small remaining magnetization induced by deviations from stoichiometry. We employed the fully-relativistic SPR-KKR (Spin-Polarized Relativistic Korringa-Kohn-Rostoker) method using the standard generalized gradient approximation Perdew et al. (1996) for the exchange-correlation potential. The structural information on MnVFeAl is taken from a recent experiment Stinshoff et al. (2017a).

Though the origins of AHE being well understood theoretically, a realistic combined first-principles description still remains a challenging computational task. At present, the most general approach for equally considering the sources of AHE is the so-called Kubo-Bastin formalism. Being implemented within the SPR-KKR method Ebert et al. (2011); Ködderitzsch et al. (2015), it allows us to deal with the charge transport in solids by treating various disorder effects on the basis of the CPA (Coherent Potential Approximation) Soven (1967); Taylor (1967).

Since the X-ray diffraction (XRD) refinement Stinshoff et al. (2017a) does not unambiguously resolve the occupancies of the and Wyckoff positions, we first specified the chemical order in the system. Most of the integral characteristics of the system, such as the magnetization, are not very sensitive to the partial ordering; however partial ordering might significantly influence the charge transport. Treating our system within the 3m symmetry, we assumed and sites were different. This allowed us to mix Mn with Fe, gradually going from the most ordered case (Mn)(Fe) (3m) to the most disordered case (MnFe)(MnFe), which has higher effective symmetry (Fm  m). Both variants are shown in Fig. 1 a and b.

Figure 1: MnVFeAl within (a) 3m (SG 216, with and Wyckoff sites occupied by Mn and Fe, respectively) and (b) Fm  m (SG 225, for which and sites become equivalent by changing to common type with random MnFe occupation). Other sites, and , occupied by MnV and Al, respectively, remain the same in both structures. Arrows indicate the spin moments of Mn atoms. (c) and (d) show the corresponding (to (a) and (b), respectively) spin-resolved (red - spin-up, blue - spin-down) spectral densities. (e) The total energy as a function of (occupation parameter), i.e., the amount of Mn in position: corresponds to (a), - to (b).

Even though their electronic structures (Fig. 1 c, d) were looking similar, increased broadening of the spin-down states was observed in the vicinity of the Fermi energy for the case (d), which was caused by the additional Mn/Fe disorder. This broadening should impose a drastic difference in the transport properties of the case (d) with respect to case (c). Calculating the total energy as a function of the occupation rate : (MnFe)(MnFe), , provided information concerning the most stable phase. As shown in Fig. 1 e, the total energy decreased monotonically with and reached its minimum at . This behavior indicates that MnVFeAl effectively has Fm  m symmetry.

Having specified the chemical order, we proceeded with the precise calibration of the Fermi energy . Again, small deviations of do not influence the integral properties as the magnetization, but might be crucial for the transport properties. These deviations can occur both in experiment (e.g., due to chemical and structural imperfections) as well as in calculations (e.g., due to the spherical approximation of the atomic potentials). For this reason, we computed both and as functions of the position (Fig. 2).

Figure 2: Residual resistivities as a function of the Fermi energy shift . (a) Longitudinal resistivity , (b) anomalous Hall resistivity . Red and blue curves correspond to the and variants; empty circles are the experimental values Stinshoff et al. (2017b) measured at low temperatures (indicated explicitly).

For we observed a strong dependence on for both and , which showed the best simultaneous agreement with experiment at  meV above the nominal . At the same time, for both quantities strongly deviated from experiment within the whole range of .

The temperature dependency of the charge transport for was examined by considering two basic sources of disorder induced by temperature: phonons and magnons. Here they are considered in an approximate way as an additional quasi-static disorder: phonons - as positional disorder, magnons - as spin-orientation disorder Ebert et al. (2015). In addition, we neglected the -dependency of the Fermi-Dirac statistics and identified the actual chemical potential with . The ability to treat both thermal disorder sources within the CPA formalism made this approach especially convenient. Even though the non-local details and the specific features of the thermal oscillatory modes are neglected, the practical use of this approach has been convincingly demonstrated Ebert et al. (2015); Chadova et al. (2017); Mankovsky et al. (2017).

The -dependency of the mean amplitude of the atomic displacements was determined here by the Debye theory (the effective Debye temperature was taken as an average over atomic types), whereas the directions of displacements were selected along the basis vectors to keep the conformity with the lattice. The atomic spins were assumed to have -independent amplitudes (; is the number of atoms in the unit cell), and thus were calculated from first principles, but the adequateness of the -dependency of their angular distribution expressed by weights, must be determined. At a fixed temperature , the angular distribution of the -th atomic spin gives its effective average value: ( is a fixed set of all possible spatial directions). The angular distribution was assumed to be Gibbs-like (see Eqs. 13-15 in Ref. Ebert et al. (2015)) with weights determined by fitting the experimental value: . Such a mapping is unique only for a single magnetic sublattice, where the experimental magnetization unambiguously defines the angular distribution of each atomic spin, since (index “z” denotes a projection on the common magnetization axis). In the present case, even though is known, the unit cell contains five different magnetic sublattices: V(), Mn(), V, Fe() and Mn(). We simplified this situation by assuming that the same form of the -dependency applies to all atomic spins that randomly share the same Wyckoff site, which reduced the number of magnetic sublattices from five to three (i.e., , and ). To avoid the remaining ambiguity, we assumed some reasonable form of the -dependency for each sublattice, e.g., by implying a sublattice-specific Bloch’s law: , where , and (playing the role of an ordering temperature for the -th sublattice) are -independent fitting parameters and - the ground-state atomic spin moments calculated from first principles. Thus, we fitted by using the following expression: , with running over three atomic sublattices entering the unit cell with the corresponding multiplicities, which are implicitly included in .

Figure 3: Experimental magnetization Stinshoff et al. (2017b) in /f.u. (black solid line) versus fit (black dashed line) together with the z-projections of the sublattice spin moments derived from the fit (red, blue and green correspond to (MnFe), (MnV) and (Al), respectively).

The fit (see Fig. 3) resulted in rather close sets for the ordering temperatures 345.6, 345.0 and 345.0 K, as well as for the power factors , 2.92 and 3.10, , 0.35 and 0.55 for sites , and , respectively. These factors appeared to have the same order of magnitude as those in the conventional Bloch’s law (, ).

The conductivities and calculated as functions of are shown in Fig. 4.

Figure 4: (a) Longitudinal and (b) anomalous Hall conductivities. Dashed green (up-triangles) and red (down-triangles) curves correspond to the case when only either magnetic fluctuation or atomic vibrations, respectively, are taken into account. The blue curve (circles) corresponds to the simultaneous inclusion of both scattering sources. Hollow squares stand for experimental values Stinshoff et al. (2017b).

The effects of spin-fluctuations and atomic vibrations are demonstrated by two additional curves, where the calculation accounts either only for spin-fluctuations (marked as “fluct.”) or only for atomic vibrations (“vib.”). These scattering sources cannot be combined, neither as parallel nor as sequential resistors (i.e., neither of these combinations gives the blue curve), even at low temperatures. On the other hand, the result based on the spin-fluctuations alone (green) followed the total curve (blue) more closely indicating that the spin disorder is the dominant scattering source. Both computed and reasonably agreed with the experimental values over the whole temperature range. The strongest deviation from experiment was simultaneously observed around 100 K for both quantities (in case of @100 K the deviation was more than 50 %, however due to , for the absolute deviation the relation holds). The main reason for the deviations are the aforementioned assumptions about the angular distribution of the spin moments, which might deviate from the actual distribution more strongly in the -range where the dispersion is already large, but the distribution is still far from uniform. The adequate description of this temperature regime becomes rather complicated, but it can be improved by systematically considering different aspects influencing the distribution of the local moments, such as the specific features of the magnon dispersion, additional angular correlations imposed by relativistic effects, and possible longitudinal spin fluctuations.

In addition to the determination of the chemical order, the present calculations explain several aspects specific to ferrimagnets, such as the directions of local moments in the magnetically compensated state. Since the reversal of local moment occurs simultaneously with the sign change of , , the moments of Mn and Fe on positions are positive (aligned along an infinitesimal small external magnetic field), whereas those of Mn and V on are negative. Further, the residual chemical disorder is shown to reduce the AHE: in the Kubo–Bastin formalism Ködderitzsch et al. (2015), the transverse conductivity is the sum of the Fermi-surface term (, the contribution from the conducting electrons at ) and the Fermi-sea term (, the contribution from the occupied states), , which appear to be large quantities with opposite sign: . This relation holds in the whole temperature range up to the magnetic critical point, where both terms simultaneously vanish (see Fig. 5 a).

Figure 5: (a) Anomalous Hall conductivities versus temperature. Red and blue curves correspond to the Fermi-surface and Fermi-sea terms. The black solid line is their sum , scaled up by a factor 50, as well as the experimental values Stinshoff et al. (2017b) (, hollow squares). (b)  vs residual magnetization . Annotated values correspond to the stoichiometric variation on site, MnV, which controls .

While is almost insensitive to the residual disorder, is strongly dependent on disorder and vanishes only close to the perfect limit, thereby increasing the total sum . However, this does not apply to the present material as it is strongly disordered.

The non-trivial observation in which the ideally compensated collinear ferrimagnet can exhibit a non-zero AHE does not unambiguously follow from the above data since neither the experimental nor the theoretical situations are ideal. Small residual magnetization is present both in experiment and in the ground-state calculations; the computed value is for the nominal (non-shifted) . The applied calibration shift  meV slightly influences further. To demonstrate the nonzero AHE at , we have adjusted the stoichiometry so that within the numerical precision (see Fig. 5 b). This can be achieved, for instance, by a slight excess of Mn on the site: MnV. Some non-zero values of are negative since we do not change the directions of the atomic moments, in order to preserve the sign of . As it follows, continuously changes with and does not show any minimum in the amplitude by approaching . Thus, the AHE should not vanish in the ferrimagnets because of magnetic compensation. We emphasize that the aspect of full compensation is rather fundamentally than technologically relevant, since it is almost impossible in practice to remove small rest of the magnetization even in antiferromagnets. On the other hand, this makes the verification of a non-vanishing AHE technically difficult, since (or ) changes its sign with the reversal of the external magnetic field and thus passes through zero Novogrudskii and Fakidov (1965); Stinshoff et al. (2017a).

To conclude, we provided an extended first-principles description of the temperature-dependent charge transport in the compensated ferrimagnet MnVFeAl, which was in good agreement with experiment. In particular, we analyzed the influence of disorder on a charge transport and proved the possibility of a non-zero anomalous Hall effect in the ideally compensated state.

References

  • MacDonald and Tsoi (2011) A. H. MacDonald and M. Tsoi, Phil. Trans. R. Soc. A 369, 3098 (2011).
  • Barthem et al. (2013) V. M. T. S. Barthem, C. V. Colin, H. Mayaffre, M.-H. Julien, and D. Givord, Nat. Commun. 4, 2892 (2013).
  • Wadley et al. (2016) P. Wadley, B. Howells, J. Železný, C. Andrews, V. Hills, R. P. Campion, V. Novák, K. Olejník, F. Maccherozzi, S. S. Dhesi, et al., Science 351, 192404 (2016).
  • van der Bijl et al. (2013) E. van der Bijl, R. E. Troncoso, and R. A. Duine, Phys. Rev. B 88, 064417 (2013).
  • Watanabe et al. (2016) H. Watanabe, K. Hoshi, and J.-I. Ohe, Phys. Rev. B 94, 125143 (2016).
  • Singh et al. (2016) S. Singh, S. W. D’Souza, J. Nayak, E. Suard, L. Chapon, A. Senyshyn, V. Petricek, Y. Skourski, M. Nicklas, C. Felser, et al., Nat. Commun. 7, 12671 (2016).
  • Kübler and Felser (2014) J. Kübler and C. Felser, Europhys. Lett. 108, 67001 (2014).
  • Feng et al. (2015) W. Feng, G.-Y. Guo, J. Zhou, Y. Yao, and Q. Niu, Phys. Rev. B 92, 144426 (2015).
  • Chadov et al. (2013) S. Chadov, J. Kiss, and C. Felser, Adv. Func. Mater. 23, 832 (2013).
  • Wollmann et al. (2015a) L. Wollmann, G. H. Fecher, S. Chadov, and C. Felser, J. Phys. D: Appl. Phys. 48, 164004 (2015a).
  • Chadov et al. (2015) S. Chadov, S. W. D’Souza, L. Wollmann, J. Kiss, G. H. Fecher, and C. Felser, Phys. Rev. B 91, 094203 (2015).
  • Chen et al. (2014) H. Chen, Q. Niu, and A. H. MacDonald, Phys. Rev. Lett. 112, 017205 (2014).
  • Kleiner (1966) W. H. Kleiner, Phys. Rev. 142, 318 (1966).
  • Seemann et al. (2015) M. Seemann, D. Ködderitzsch, S. Wimmer, and H. Ebert, Phys. Rev. B 92, 155138 (2015).
  • Slater (1936) J. C. Slater, Phys. Rev. 49, 931 (1936).
  • Pauling (1938) L. Pauling, Phys. Rev. 54, 899 (1938).
  • Li et al. (2013) G. J. Li, E. K. Liu, Y. J. Zhang, Y. Du, H. W. Zhang, W. H. Wang, and G. H. Wu, J. Appl. Phys. 113, 103903 (2013).
  • Wollmann et al. (2015b) L. Wollmann, S. Chadov, J. Kübler, and C. Felser, Phys. Rev. B 92, 064417 (2015b).
  • Nayak et al. (2015) A. K. Nayak, M. Nicklas, S. Chadov, P. Khuntia, C. Shekhar, A. Kalache, M. Baenitz, Y. Skourski, V. K. Guduru, A. Puri, et al., Nat. Mater. 14, 679 (2015).
  • Stinshoff et al. (2017a) R. Stinshoff, A. K. Nayak, G. H. Fecher, B. Balke, S. Ouardi, Y. Skourski, T. Nakamura, and C. Felser, Phys. Rev. B 95, 060410 (2017a).
  • Stinshoff et al. (2017b) R. Stinshoff, G. H. Fecher, S. Chadov, A. K. Nayak, B. Balke, S. Ouardi, T. Nakamura, and C. Felser, accepted in AIP Advances (2017b).
  • Perdew et al. (1996) J. P. Perdew, K. Burke, and M. Ernzerhof, Phys. Rev. Lett. 77, 3865 (1996).
  • Ebert et al. (2011) H. Ebert, D. Ködderitzsch, and J. Minár, Rep. Prog. Phys. 74, 096501 (2011).
  • Ködderitzsch et al. (2015) D. Ködderitzsch, K. Chadova, and H. Ebert, Phys. Rev. B 92, 184415 (2015).
  • Soven (1967) P. Soven, Phys. Rev. 156, 809 (1967).
  • Taylor (1967) D. W. Taylor, Phys. Rev. 156, 1017 (1967).
  • Ebert et al. (2015) H. Ebert, S. Mankovsky, K. Chadova, S. Polesya, J. Minár, and D. Ködderitzsch, Phys. Rev. B 91, 165132 (2015).
  • Chadova et al. (2017) K. Chadova, S. Mankovsky, J. Minár, and H. Ebert, Phys. Rev. B 95, 125109 (2017).
  • Mankovsky et al. (2017) S. Mankovsky, S. Polesya, K. Chadova, H. Ebert, J. B. Staunton, T. Gruenbaum, M. A. W. Schoen, C. H. Back, X. Z. Chen, and C. Song, Phys. Rev. B 95, 155139 (2017).
  • Novogrudskii and Fakidov (1965) V. N. Novogrudskii and I. G. Fakidov, Sov. Phys. J.E.T.P. 47, 20 (1965).
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