Spin battery operated by ferromagnetic resonance, Notas de estudo de Engenharia de Produção
igor-donini-9
igor-donini-9

Spin battery operated by ferromagnetic resonance, Notas de estudo de Engenharia de Produção

4 páginas
10Números de download
1000+Número de visitas
Descrição
Spin battery operated by ferromagnetic resonance
20 pontos
Pontos de download necessários para baixar
este documento
Baixar o documento
Pré-visualização3 páginas / 4
Esta é apenas uma pré-visualização
3 mostrados em 4 páginas
Esta é apenas uma pré-visualização
3 mostrados em 4 páginas
Esta é apenas uma pré-visualização
3 mostrados em 4 páginas
Esta é apenas uma pré-visualização
3 mostrados em 4 páginas

RAPID COMMUNICATIONS

PHYSICAL REVIEW B 66, 060404~R! ~2002!

Spin battery operated by ferromagnetic resonance

Arne Brataas,1 Yaroslav Tserkovnyak,1 Gerrit E. W. Bauer,2 and Bertrand I. Halperin1 1Harvard University, Lyman Laboratory of Physics, Cambridge, Massachusetts 02138

2Department of Applied Physics and DIMES, Delft University of Technology, 2628 CJ Delft, The Netherlands ~Received 1 May 2002; published 29 August 2002!

Precessing ferromagnets are predicted to inject a spin current into adjacent conductors via Ohmic contacts, irrespective of a conductance mismatch with, for example, doped semiconductors. This opens the way to create a pure spin source ~‘‘spin battery’’! by the ferromagnetic resonance. We estimate the spin current and spin bias for different material combinations.

DOI: 10.1103/PhysRevB.66.060404 PACS number~s!: 76.50.1g, 72.25.Mk, 73.23.2b, 73.40.2c

The research field of magnetoelectronics or spinelectron- ics strives to utilize the spin degree of freedom for electronic applications.1 Devices made from metallic layered systems displaying the giant2 and tunnel magnetoresistance3 have been proven useful for read-head sensors and magnetic random-access memories. Integration of such devices with semiconductor electronics is desirable but difficult because a large resistivity mismatch between magnetic and normal ma- terials is detrimental to spin injection.4 Spin injection into bulk semiconductors has been reported only in optical pump and probe experiments,5 and with high-resistance ferromag- netic injectors6 or Schottky/tunnel barriers.7 In these cases, the injected spin-polarized carriers are hot and currents are small. Desirable are semiconductor devices with an efficient all-electrical cold-electron spin injection and detection via Ohmic contacts at the Fermi energy, just as has been realized by Jedema et al. for metallic devices.8

We introduce a concept for dc spin-current injection into arbitrary conductors through Ohmic contacts, which does not involve net charge currents. The spin source is a ferromag- netic reservoir at resonance with an rf field. Pure spin-current injection into low-density conductors should allow experi- mental studies of spintronic phenomena in mesoscopic, bal- listic, and nanoscale systems, which up to now has been largely a playground of theoreticians like Datta and Das,9

whose spin transistor concept has stimulated much of the present interest in spintronics.

The combination of a ferromagnet at the ferromagnetic resonance ~FMR! in Ohmic contact with a conductor can be interpreted as a ‘‘spin battery,’’ with analogies and differ- ences with charge batteries. For example, charge-current conservation dictates that a charge battery has two poles, plus and minus. A spin battery requires only one pole, since the spin current does not need to be conserved. Furthermore, the polarity is not a binary, but a three-dimensional vector. The important parameters of a charge battery are the maxi- mum voltage in the absence of a load, as well as the maxi- mum charge current, which can be drawn from it. In the following we present estimates for the analogous character- istics of the spin battery.

Central to our concept is a precessing ferromagnet, which acts as a source of spin angular momentum, when in contact with normal metals,10 see Fig. 1. This spin injection can be formulated in analogy with the adiabatic pumping of charge in mesoscopic systems.11,12 When the ferromagnet is thicker

0163-1829/2002/66~6!/060404~4!/$20.00 66 0604

than the ferromagnetic coherence length ~a few Å in transi- tion metals such as Co, Ni, or Fe!, the spin current emitted into the normal metal is determined by the mixing conductance12 g↑↓5(nm@dnm2rnm

(rnm ↓ )*# in terms of the

spin-dependent reflection amplitudes rnm ↑() between trans-

verse modes m and n in the normal metal at the interface to the ferromagnet, where the latter is characterized by the mag- netization direction m. The mixing conductance governs the transport of spins that are noncollinear to the magnetization direction in the ferromagnet12,13 and is also a material param- eter proportional to the torque acting on the ferromagnet in the presence of a noncollinear spin accumulation in the nor- mal metal.10,12,14,15 For most systems ~with the exception of, e.g., ferromagnetic insulators16! the imaginary part of the mixing conductance can be disregarded due to the random- ization of phases of spin-up and spin-down electrons in re- ciprocal space14 and this is assumed in the following. The spin current emitted into the normal metal is then, simply,10

Is source5

\

4p g↑↓m3

dm

dt . ~1!

In our notation, the spin current is measured in units of me- chanical torque. Equation ~1! is a time-dependent correction to the Landauer-Büttiker formula for noncollinear ferromagnetic–normal-metal (F-N) hybrid systems.12 A simple physical picture can be inferred from the following thought experiment.17 Suppose we have a F-N interface at

FIG. 1. Schematic view of the spin battery. Precession of the magnetization m(t) of the ferromagnet F emits a spin current Is

source

into the adjacent normal-metal layer N. The spin accumulation in the normal metal either relaxes by spin-flip scattering or flows back into the ferromagnet, resulting in a net spin current Is5Is

source

2Is back .

©2002 The American Physical Society04-1

RAPID COMMUNICATIONS

BRATAAS, TSERKOVNYAK, BAUER, AND HALPERIN PHYSICAL REVIEW B 66, 060404~R! ~2002!

equilibrium and switch the magnetization instantaneously. The mismatch of the spin-up and spin-down chemical poten- tials leads to large nonequilibrium spin currents on the length scale of the spin-diffusion length. A slower magnetization reversal naturally induces smaller spin currents. Equation ~1! represents the adiabatic limit of the spin currents pumped by a slow magnetization dynamics. When the spin current ~1! is channeled off sufficiently rapidly, the corresponding loss of angular momentum increases the ~Gilbert! damping of the magnetization dynamics.10 Equation ~1! is the maximum spin current that can be drawn from the spin battery.

Next, we need the maximum spin bias obtained when the load vanishes. When the spin-flip relaxation rate is smaller than the spin-injection rate, a spin angular momentum s ~in units of \) builds up in the normal metal. We can neglect spatical dependence within the ferromagnet when the film is sufficiently thin.18 Under these conditions, one finds that the component of the backflow spin current Is

back , from the nor- mal metal to the ferromagnet, parallel to the instantenous magnetization direction m is cancelled by an opposite flow from the ferromagnet. The componenent of Is

back perpendicu- lar to m is12

Is back5

g↑↓ 2pN

@s2m~ms!# , ~2!

where N is the one-spin density of states. We note that the mixing conductance in Eqs. ~1! and ~2! ought to be renor- malized in highly transparent junctions.19

The relation between spin excess s and total spin current Is5Is

source2Is back in a normal diffusive metal is governed by

the spin-diffusion equation20

]s

]t 5D

]2s

]x2 2

s

ts , ~3!

where D is the diffusion coefficient, in three ~two! dimen- sions D5vF

2 t/6 (D5vF 2 t/4), and t ,ts are the elastic and

spin-flip relaxation times, respectively. We solve the diffu- sion equation with boundary conditions at x50, where (DA\)]xs52Is and at the end of the sample x5L , where the spin current vanishes, ]xs50. A is the cross section of the system.

The precession of the magnetization vector of a ferromag- net under a resonant rf electromagnetic field applied perpen- dicularly to a dc magnetic field21 can be used to drive the spin battery. The magnitude of the spin current Is

source and spin bias Dm[2^s& t /N as a function of the applied field H0 follows from the Landau-Lifshitz-Gilbert equation ṁ5 2g*m3H01am3ṁ, where g* is the gyromagnetic ratio, a;0.0120.001 the Gilbert damping factor, and magnetic anisotropies have been disregarded for simplicity. The spin bias also has ac components. However, its frequency v har- monics are strongly suppressed when ls /(vts)

1/2,L,ls , which can be easily realized when vts.1, e.g., ts.v

21

;10211s/H0 (T). ls5ADts is the spin-diffusion length in the normal metal. The dominant contribution to the spin bias is then constant in time and directed along H0. The magni-

06040

tude of the time-averaged spin accumulation Dm [2^s(t)& t /N in the normal metal close to the F-N interface then reads

Dm5\v0 sin2u

sin2u1h , ~4!

where the precession cone angle between H0 and m is u ,h 5(t i /ts)tanh(L/ls)/(L/ls) is a reduction factor, and we have introduced the spin-injection rate t i

215g↑↓ /(2p\NAL). Large systems have a smaller injection rate since more states have to be filled.

The ratio of the injection and spin-flip relaxation times can be evaluated for a planar geometry. We consider a free- electron gas in contact with a metallic ferromagnet. The mix- ing conductance is g↑↓5kAkF

2 /(4p)(g↑↓5kAkF /p) for spin injection into three-~two-!dimensional systems. First- principles band-structure calculations show that for combina- tions like Co/Cu or Fe/Cr, k remains close to unity.14 The ratio between the injection and spin-flip relaxation times in three ~two! dimensions can be calculated to be t i /ts 5A8/3k21Ae(L/ls) @t i /ts52k21Ae(L/ls)# . e5t/ts is the ratio of the elastic scattering rate and the spin-flip relaxation rate, which is usually much smaller than unity.

When the spin relaxation time is longer than the spin in- jection time and the precession cone angle is sufficiently large, sin2u.h, the spin bias saturates at its maximum value Dm05\v0. In this regime the spin accumulation does not depend on the material parameters. It should be feasible to realize the full spin bias when L!ls since h 'A8/3k21Ae(L/ls), e.g., when L/ls50.1, A8/3k21Ae 50.1 the precession cone angle should be larger than 6°. For small precession cone angles u'H1 /(aH0), so, for ex- ample, H051.0 T,a510

23 this requires a H150.1 mT rf field with a resulting spin bias of Dm50.1 meV. For a smaller precession angle, e.g., u50.6° the spin bias is smaller, Dm51 mV, but still clearly measurable. Epitaxially grown clean samples with even longer spin-diffusion lengths and smaller spin-flip to non-spin-flip relaxation ratios e will function as spin batteries with smaller precession angles. The precession cone angle u in FMR is typically small, but u .15° can be achieved for a sufficiently intense rf field and a soft ferromagnet, e.g., permalloy.22 The maximum dc spin current source is u^Is

source& tu'\v0kAkF 2 sin2u/(4p), e.g., for a

precession cone angle of u56° the equivalent electrical spin current (e/\)u^Is

source& tu is 0.1 nA per conducting channel AkF

2 /(4p). The total number of channels is a large number since the cross sections may be chosen very much larger than the Fermi wavelength thus ensuring that a large spin current may be drawn from the battery.

Ferromagnetic resonance dissipates energy proportional to the damping parameter a of the magnetization dynamics. The power loss dE/dt5a\v0

2Nssin 2u is proportional to the

volume of the ferromagnet through the number of spins in the ferromagnet in units of \ ,Ns . The power loss can be significant even for a thin film ferromagnet, e.g., for a 10 monolayer thick Fe film with a;1023,sin2u;1022, and v0;10

11 s21, the power loss per unit area is (1/A)dE/dt

4-2

RAPID COMMUNICATIONS

SPIN BATTERY OPERATED BY FERROMAGNETIC RESONANCE PHYSICAL REVIEW B 66, 060404~R! ~2002!

;0.1 W/cm2. The temperature can be kept low by, e.g., im- mersing the sample in superfluid helium. The heat transfer is then approximately 8 W/cm2 K for small temperature gradi- ents and increases for larger temperature gradients,23 which appears sufficient for the present purpose.

Schmidt et al.4 realized that efficient spin injection into semiconductors by Ohmic contacts is close to impossible with transition-metal ferromagnets since virtually all of the applied potential drops over the nonmagnetic part and is wasted for spin injection. The present mechanism does not rely on an applied bias and does not suffer from the conduc- tance mismatch, because the smallness of the mixing con- ductance for a ferromagnet-semiconductor interface is com- pensated by the small spin current that is necessary to saturate the spin accumulation.

Possible undesirable spin precession and energy genera- tion in the normal-metal parts of the system is of no concern for material combinations with different g factors, as, e.g., Fe (g52.1) and GaAs (g520.4), or when the magnetic an- isotropy modifies the resonance frequency with respect to electrons in the normal metal.

The optimal material combinations for a battery depend on the planned usage. From Eq. ~1! it follows that the largest spin current can be achieved when the conductor is a normal metal, whereas any material combination appears suitable when the load is small, as long as the contact is Ohmic and the system is smaller than the spin-diffusion length.

Standard metals, such as Al and Cu, are good candidate materials, since the spin-diffusion length is very long, ls ;1 mm at low temperatures, and remains quite long at room temperature.8,24 Indirect indications of spin accumulation in Cu can be deduced from the absence of any enhancement of the Gilbert damping in FMR when in contact with thin fer- romagnetic films.10,25

Semiconductors have the advantage of a larger ratio of spin bias to Fermi energy. Let us first consider the case of GaAs. The spin-flip relaxation time in GaAs can be very long, ts510

27 s at n5531016 cm3 carrier density.26 These favorable numbers are offset by the difficulty to form Ohmic contacts to GaAs, however. Large Schottky barrier exponentially suppress the interfaces mixing conductance parameter k .

InAs has the advantage of a natural accumulation layer at the surface that avoids Schottky barriers when covered by high-density metals. However, the spin-orbit interaction in a narrow gap semiconductor like InAs is substantial, which reduces ts . In asymmetric confinement structures, the spin- flip relaxation rate is governed by the Rashba type spin-orbit interaction, which vanishes in symmetrical quantum wells.27

The remaining D’yakonov-Perel scattering rate is reduced in narrow quasi-one-dimensional channels of width d due to waveguide diffusion modes by a factor of (Ls /d)

2, where Ls5vF /uh(kF)u is the spin-precession length in terms of the spin-orbit coupling Hso5h(k)•s,

28 which makes InAs based systems an interesting material for a spin battery as well.

In Si, the spin-flip relaxation time is long, since spin-orbit interaction is weak. Furthermore, the possibility of heavy doping allows control of Schottky barriers. So, Si appears to be a good candidate for spin injection into semiconductors.

06040

The spin bias can be detected noninvasively via tunnel junctions with an analyzing ferromagnet having a switchable magnetization direction. A voltage difference of pDm is de- tected for parallel and antiparallel configurations of the ana- lyzing magnetization with respect to the spin accumulation in the normal metal, where p5(G↑2G↓)/(G↑1G↓) is the relative polarization of the tunnel conductances of the con- tact. The test magnetic layer need not be flipped. It is suffi- cient to reverse the direction of the dc static magnetic field. The spin current, however, can be measured via the drop of spin bias over a known resistive element.

Spin pumping into the normal metal can also have conse- quences for the nuclei via the hyperfine interaction between electrons and nuclear spins.26 An initially unpolarized collec- tion of nuclear spins can be oriented by a spin-polarized electron current, which transfers angular momentum by spin- flop scattering. A ferromagnetically ordered nuclear-spin sys- tem can lead to an Overhauser29 field on the electron spin. This effect does not affect the spin bias Dm, but induces an equilibrium spin density in the normal metal s0 via the nuclear magnetic field, and can be exploited in experiments where the the total spin-density s1s0 is an important param- eter. The electron-nuclear interaction can be included by adding21,29

Is nuc5

\sn Tn

~5!

to the electron spin dynamics so that IIssource2Isback1Isnuc , where sn is the nonequilibrium nuclear spin accumulation and Tn is the electron-nuclear relaxation time. The nuclear spin dynamics is described by

dsn dt

52 sn Tn8

1 s

Te , ~6!

where Tn8<Tn is the nuclear-spin relaxation time and Te is the nuclear-electron relaxation. In steady state, sn5(Tn8/Tn) 3(Tn /Te)s. In the experimentally relevant regime Te

21

!t i 21 the electron-nuclear interaction ~5! has a negligible

effect on the nonequilibrium spin accumulation s and thus Eq. ~4! remains unchanged. Tn /Te58I(I11)eFnN / (9kBTne) for small polarizations, where eF is the Fermi en- ergy of the electron gas, kBT is the thermal energy, nN is the nuclear density, and ne is the one-spin electron density.

29

Using N5(3/2)ne /eF (N5ne /eF in two dimensions! and Eq. ~4! the relative enhancement of the dc nuclear spin po- larization is

sn5nN Tn8

Tn

2

3 I~I11 !

Dm

kBT , ~7!

for Dm!kBT . The nuclear-spin polarization increases with the spin bias and by lowering the temperature. The hyperpo- larized nuclei, in turn, produce an effective nuclear field that polarizes the equilibrium properties of the electron gas s0. In bulk GaAs, the nuclear magnetic field is Bn55.3 T when the nuclei are fully spin polarized, which should occur at suffi- ciently low temperatures.30

4-3

RAPID COMMUNICATIONS

BRATAAS, TSERKOVNYAK, BAUER, AND HALPERIN PHYSICAL REVIEW B 66, 060404~R! ~2002!

Berger31 proposed to generate a dc voltage by the FMR, which bears similarities with our proposal. But Berger’s mechanism of spin injection, originating from the spin-flip scattering in the ferromagnet as induced by spin waves ap- pears to be different from ours. We propose to achieve spin injection via the modulation of the interface scattering matrix by the coherent precession of the magnetization, which al- lows, for example, quantitative calculations for various ma- terials.

In conclusion, we present the concept of a spin battery, which is a source of spin, just as a conventional battery is a

06040

source of charge, and estimate its performance for different material combinations.

We are grateful to I. Appeli, B. Heinrich, A. D. Kent, D. Monsma, and H. C. Siegmann for stimulating discussions. This work was supported in part by the DARPA award No. MDA 972-01-1-0024, the NEDO International Joint Re- search Grant Program ‘‘ Nanomagnetoelectronics,’’ FOM, the Schlumberger Foundation, and NSF Grant No. DMR 99-81283. G. E. W. B. acknowledges the hospitality of Dr. Y. Hirayama and his group at the NTT Basic Research Laboratories.

1 S. Wolf, D.D. Awschalom, R. Buhrman, J. Daughton, S. von Mol- nar, M. Roukes, A. Chtchelkanova, and D. Treger, Science 294, 1488 ~2001!.

2 M. Baibich, J.M. Broto, A. Fert, F.N.V. Dau, F. Petroff, P. Eitenne, G. Creuzet, A. Friederich, and J. Chazelas, Phys. Rev. Lett. 61, 2472 ~1988!.

3 T. Miyazaki and N. Tezuka, J. Magn. Magn. Mater. 139, L231 ~1995!; J.S. Moodera, L.R. Kinder, T.M. Wong, and R. Meservey, Phys. Rev. Lett. 74, 3273 ~1995!.

4 G. Schmidt, D. Ferrand, L.W. Molenkamp, A.T. Filip, and B.J. van Wees, Phys. Rev. B 62, R4790 ~2000!.

5 J.M. Kikkawa and D.D. Awschalom, Nature ~London! 397, 139 ~1999!.

6 R. Fiederling, M. Keim, G. Reuscher, W. Ossau, G. Schmidt, A. Waag, and L.W. Molenkamp, Nature ~London! 402, 787 ~1999!; Y. Ohno, D.K. Young, B. Beschoten, F. Matsukura, H. Ohno, and D.D. Awschalom, ibid. 402, 790 ~1999!.

7 D. Monsma, R. Vlutters, and J. Lodder, Science 281, 407 ~1998!; H.J. Zhu, M. Ramsteiner, H. Kostial, M. Wassermeier, H.-P. Schonherr, and K.H. Ploog, Phys. Rev. Lett. 87, 016601 ~2001!; A. T. Hanbicki, B. T. Jonker, G. Itskos, G. Kioseoglou, and A. Petrou, Appl. Phys. Lett. 80, 1240 ~2002!; V. Motsnyi, V. Safa- rov, J.D. Boeck, W.v.R.J. Das, E. Goovaerts, and G. Borghs, cond-mat/0110240 ~unpublished!; S. Parkin ~unpublished!.

8 F.F. Jedema, A.T. Filip, and B.J. van Wees, Nature ~London! 410, 345 ~2001!.

9 S. Datta and B. Das, Appl. Phys. Lett. 56, 665 ~1990!. 10 Y. Tserkovnyak, A. Brataas, and G.E.W. Bauer, Phys. Rev. Lett.

88, 117601 ~2002!. 11 P.W. Brouwer, Phys. Rev. B 58, R10135 ~1998!. 12 A. Brataas, Y.V. Nazarov, and G.E.W. Bauer, Phys. Rev. Lett. 84,

2481 ~2000!; Eur. Phys. J. B 22, 99 ~2001!. 13 D. Huertas-Hernando, Y.V. Nazarov, A. Brataas, and G.E.W.

Bauer, Phys. Rev. B 62, 5700 ~2000!. 14 K. Xia, P.J. Kelly, G.E.W. Bauer, A. Brataas, and I. Turek, Phys.

Rev. B 65, 220401~R! ~2002!. 15 M.D. Stiles and A. Zangwill, Phys. Rev. B 66, 014407 ~2002!.

16 D. Huertas-Hernando, Y.V. Nazarov, and W. Belzig, Phys. Rev. Lett. 88, 047003 ~2002!.

17 This argument is attributed to H. C. Siegmann. 18 We require that the ferromagnetic film is thinner than the spin-

diffusion length and lF(J/\v0), where J is the exchange ~stiff- ness! energy, v0 is the rf frequency, and lF is the Fermi wave- length.

19 G.E.W. Bauer, Y. Tserkovnyak, D. Huertas-Hernando, A. Brataas, cond-mat/0205453 ~unpublished!; K.M. Schep, J.B.A.N. van Hoof, P.J. Kelly, G.E.W. Bauer, and J.E. Inglesfield, Phys. Rev. B 56, 10 805 ~1997!.

20 M. Johnson and R.H. Silsbee, Phys. Rev. B 37, 5312 ~2000!. 21 C. P. Slichter, Principles of Magnetic Resonance, 3rd ed.

~Springer-Verlag, NY, 1990!. 22 B. Heinrich, ~private communication!. 23 W.J. Skocpol, M.R. Beasley, and M. Tinkham, J. Appl. Phys. 45,

4054 ~1974!. 24 F. J. Jedema, H. B. Heershce, A. T. Filip, J. J. A. Baselmans, and

B. J. van Wees, Nature ~London! 416, 713 ~2002!. 25 S. Mizukami, Y. Ando, and T. Miyazaki, J. Magn. Magn. Mater.

226, 1640 ~2001!; S. Mizukami, Y. Ando, and T. Miyazaki, Jpn. J. Appl. Phys. 40, 580 ~2001!.

26 R.K. Kawakami, Y. Kato, M. Hanson, I. Malajovich, J.M. Stephens, E. Johnston-Halperin, G. Salis, A.C. Gossard, and D.D. Awschalom, Science 294, 131 ~2001!; J.H. Smet, R.A. Deutschmann, F. Ertl, W. Wegscheider, G. Abstreiter, and K. von Klitzing, Nature ~London! 415, 281 ~2002!; K. Hashimoto, K. Muraki, T. Saku, and Y. Hirayama, Phys. Rev. Lett. 88, 176601 ~2002!.

27 J. Nitta, T. Akazaki, H. Takayanagi, and T. Enoki, Phys. Rev. Lett. 78, 1335 ~1997!; G. Engels, J. Lange, T. Schäpers, and H. Lüth, Phys. Rev. B 55, R1958 ~1997!.

28 A.G. Mal’shukov and K.A. Chao, Phys. Rev. B 61, R2413 ~2000!. 29 A.W. Overhauser, Phys. Rev. 92, 411 ~1953!. 30 D. Paget, G. Lampel, B. Sapoval, and V.I. Safarov, Phys. Rev. 15,

5780 ~1977!. 31 L. Berger, Phys. Rev. B 59, 11 465 ~1999!; J. Appl. Phys. 90,

4632 ~2001!.

4-4

Até o momento nenhum comentário
Esta é apenas uma pré-visualização
3 mostrados em 4 páginas