Spintronic magnetic anisotropy

Spintronic magnetic anisotropy

An attractive feature of magnetic adatoms and molecules for nanoscale applications is their superparamagnetism, the preferred alignment of their spin along an easy axis preventing undesired spin reversal. The underlying magnetic anisotropy barrier – a quadrupolar energy splitting – is internally generated by spin-orbit interaction and can nowadays be probed by electronic transport. Here we predict that in a much broader class of quantum-dot systems with spin larger than one-half, superparamagnetism may arise without spin-orbit interaction: by attaching ferromagnets a spintronic exchange field of quadrupolar nature is generated locally. It can be observed in conductance measurements and surprisingly leads to enhanced spin filtering even in a state with zero average spin. Analogously to the spintronic dipolar exchange field, responsible for a local spin torque, the effect is susceptible to electric control and increases with tunnel coupling as well as with spin polarization.

The growing interest in nanomagnets, e.g., magnetic adatoms (1) and single-molecule magnets (2) is fueled by prospects of their application in novel spintronic devices whose functionality derives from their unique magnetic features (3). A key property of such systems is their strong magnetic anisotropy leading to magnetic bistability, required for building blocks for nanoscale memory cells (4); (5) and non-trivial quantum dynamics, useful for quantum information processing (6); (7). In either case, operational stability of such devices hinges heavily on the height of the energy barrier opposing the spin reversal. Though recently progress in the control over the magnetic anisotropy by synthesis (8), mechanical straining (9), atomic manipulation (10) or electrical gating (11) has been made, achieving of a high spin-reversal barrier still remains a challenge. Incorporating a nanomagnet into an electronic circuit may significantly alter its magnetic properties (12); (13); (14), but may also be advantageous. One possible, spintronic route for manipulation of nanomagnets entails ferromagnetic electrodes and uses the spin torque due to spin-polarized scattering (15) or Coulomb interaction (16), magnetic analogs of the proximity effect in superconducting junctions. In this article, we present another route that combines spintronics with molecular magnetism: high-spin quantum dots can acquire a significant magnetic anisotropy that is purely of spintronic origin, instead of deriving from the spin-orbit interaction, as the tunneling to ferromagnets induces a local, quadrupolar exchange field. Besides providing an alternative approach to electrical manipulation and engineering of superparamagnetic nanomagnets, this new quantity is of key importance for the analysis of experiments that probe atoms or molecules using highly spin-polarized electrodes.

Figure 1: The origin of magnetic anisotropy splitting of a high-spin ground multiplet. a, The atomic case, a spin-1 multiplet with quenched orbital moment with virtual spin-orbit scattering into an excited state. b, The spintronic case, a spin-1 quantum dot with virtual electron tunneling into an attached ferromagnet. c, Generic model of a high-spin quantum-dot spin valve (see Methods).
Figure 2: Effective exchange fields. (Real-time perturbation theory) a, Dipolar and quadrupolar exchange fields as a function of the quantum dot level position ( gate voltage) at zero bias voltage. Parameters: eV, meV, , and . b, Excitation spectrum of a nanomagnet around the symmetry point as generated by the magnetic proximity effect.
Figure 3: Spectroscopic features of spintronic anisotropy. (DM-NRG) Dependence of the differential conductance at , approximated by the equilibrium spectral function , on the energy and the level position close to the center of the Coulomb blockade regime, . a-b, Spectral function for parallel ferromagnets with spin polarization coupled to a spin single-level quantum dot () in a, and a spin quantum dot () in b. Dashed lines in b represent the gap (see Fig. 2b and supplementary figure S-2). c-d, For the case relevant -cross-sections for several different values of the tunnel coupling (c) and the spin polarization of the ferromagnets (d) are shown. In both c and d, the left/right side of the -axis corresponds to the regime dominated by the quadrupolar field, , and the dipolar field, , respectively. Parameters: eV, meV, , , and in (a)-(b) .

Dipolar vs. quadrupolar exchange field

The origin of superparamagnetism, usually dominating the magnetic behaviour of a nanomagnet, is a magnetic anisotropy energy barrier. For instance, an adatom with a spin-degenerate ground multiplet (quenched orbital moment), is described by the generic spin Hamiltonian (2)

(1)

where denotes the component of the total spin () along the -axis, and is a diagonal component of the spin-quadrupole moment tensor. Moreover, and are dipolar and quadrupolar fields, respectively. All parameters are in units of energy (). If , the quadrupolar term prefers the axial spin states over the planar ones, i.e. the spin is aligned with the -axis but without favouring a particular orientation along it. For spin the corresponding energy splitting is sketched in Fig. 1a. At temperatures , it prevents transitions between the axial spin states via an intermediate planar state (i.e. spin reversal), while maintaining the former ones as ground states. This superparamagnetism is thus of major interest for applications in which the axial states represent an information bit, and such transitions are unwanted. On the contrary, the first term in equation (1), coupling the spin dipole to the external magnetic field (chosen along the -axis), does introduce a distinction between the ‘up’ and ‘down’ axial states. The crucial role of the -axis stems from the second term of equation (1). It emerges (2) when taking into account virtual scattering within the ground state multiplet of the adatom through the high-energy excited state at energy , caused by the spin-orbit interaction see Fig. 1a. Often, only one component of orbital angular momentum has non-zero matrix elements due to ligand-field hybridization and an uniaxial intrinsic anisotropy along the -axis is imposed by the negative . Hence, by probing the ligand environment, the atomic electrons experience a broken spin symmetry.

In spintronics a very similar situation, depicted in Fig. 1b, arises in a completely different physical setting where spin-orbit interaction is negligible. Electrons localized in a high-spin (), spin-isotropic quantum dot probe the broken spin symmetry in attached ferromagnets by virtual charge fluctuations. These fluctuations result in a spin current, which transfers spin angular momentum from the electrode to the quantum dot, resulting in a spin torque. It can be described by replacing the externally applied magnetic field in equation (1) by an effective exchange field. Specifically, we consider the setup outlined in Fig. 1c: a quantum dot with a triplet ground state obtained by coupling an orbital level via Heisenberg interaction to an immobile, spin-one-half impurity, causing a singlet-triplet splitting . The orbital level is additionally tunnel-coupled to the ferromagnets. None of the simplifying assumptions made on the impurity, namely its immobility and its low spin value, is crucial for what follows, see Supplementary Information. The physics can be understood by first ignoring the second ferromagnet. Then, the dipolar exchange field to the leading order in the tunneling rate decomposes into a difference of two contributions and  (17):

(2)

with standing for the principal value integral. Here, , and is the dot level relative to the electrochemical potential of the ferromagnet, tunable by the gate voltage. Furthermore, is the local Coulomb interaction in the dot, is the spin polarization of the ferromagnet, and denotes the half-width of the conduction band. Notably, the exchange field, plotted in Fig. 2a, depends on the gate voltage in an antisymmetric way, , reversing its sign at the symmetry point . The electron- () and hole-type () fluctuations cancel there, as experimentally observed by Hauptmann et al. (18). This is a generic feature of interacting quantum-dot spin-valves (19) if spin-polarization effects of the ferromagnets dominate (20). Approaching the symmetry point, deep in the Coulomb blockade, processes of higher order in become increasingly important. These are responsible for inelastic tunneling, as well as the Kondo effect, both being primary experimental tools in atomic-scale spin detection (21); (22); (23) and manipulation (5). The interplay of such processes with the exchange field has been analyzed (24); (19) and experimentally demonstrated for molecular (25) and carbon-nanotube (18); (20) quantum dots.

However, for high-spin quantum dots these processes result in a drastically different situation as we now explain. For our quantum dot example processes of the order , apart from inessential renormalization of , generate an additional spintronic anisotropy term of the same form as the second term of equation (1). The result for the quadrupolar exchange field (see Methods) is plotted in Fig. 2a. It takes a simple, approximate form in the regime when we neglect the excited singlet state at energy and assume a large band width [as was also done in deriving equation (2)]:

(3)

The corresponding term in equation (1) generates a quadrupolar splitting. We find that in the Coulomb blockade regime this parameter is negative, i.e. the energy of the triplet axial spin states is lowered relative to the planar spin state , as in Fig. 1b. This is entirely analogous to the uniaxial spin anisotropy typical to magnetic adatoms or molecules, cf. Fig. 1a. However, this anisotropy is induced by the proximity of the ferromagnet and displays the characteristic properties of a spintronic exchange field: it is electrically tunable by the gate voltage as shown in Fig. 2a, and scales as . It is thus enhanced with increasing tunnel coupling , similar to the Kondo effect (see below), but in contrast, it is also enhanced with increasing spin polarization , which suppresses the Kondo effect.

Importantly, Fig. 2a demonstrates that the quadrupolar field is a symmetric function of the gate voltage, , and therefore does not necessarily vanish at the symmetry point [the electron and hole contributions to equation (3) add up, unlike in equation (2)]. Expanding and linearly around the symmetry point,

(4)
(5)

we thus obtain an all-spintronic superparamagnet described by equation (1) with a constant anisotropy and a magnetic field that is linearly tunable by the gate voltage through , see Fig. 2b. Close to the symmetry point, the quadrupolar field dominates over the dipolar one in the gate voltage range proportional to the width of the low-temperature Coulomb peaks. Accordingly, high-spin quantum dot spin valves exhibit a tunable interplay of spintronics and nanomagnetism that is not possible for low-spin quantum dots. This, in turn, opens the possibility for fast all-electric operations involving the spin, which are challenging for adatoms and single-molecule magnets.

Spectral signatures of spintronic quadrupolar splittings

Based on the perturbative results (4)-(5) we expect a clear experimental transport signature of the spintronic quadrupolar field for strong tunnel coupling . The above considerations are readily extended to the case of a junction of two ferromagnets with voltage bias and parallel polarizations (see Methods). The spintronic fields and now also acquire a dependence on the bias voltage, which is, however, negligible in the situation under discussion (see Supplementary Information). In order to address the strong tunneling regime and to better estimate the achievable magnitude of we calculate the equilibrium, spin-resolved local density of states (LDOS) using the exact density-matrix numerical renormalization group (DM-NRG) method. This allows us to compute transport characteristics, while (i) including the singlet excited state at finite energy that we neglected so far, and (ii) taking into account the Kondo effect, which also gains importance with increasing at low temperature.

To set the stage, we show in Fig. 3a the result for a spin quantum-dot spin valve model (obtained by setting ), successfully used to analyse the spectroscopy of the dipolar exchange field (18); (20). Unlike for non-magnetic electrodes, a Kondo peak forms only at the symmetry point where the exchange field induced by the ferromagnets vanishes (26); (24); (19). The finite-temperature precursor of the Kondo peak in Fig. 3a displays the measured, gate-voltage dependent splitting (18).

For a high-spin ground state (i.e. ), instead of a peak, we find in Fig. 3b a pronounced gap, which linearly increases as the gate voltage is detuned from the symmetry point. This indicates a definite spin excitation, even close to the symmetry point where the influence of a dipolar exchange field on the high-spin quantum dot is negligible. As illustrated in Fig. 2b, the observed excitation as a function of is the telltale signature of uniaxial spin anisotropy of the type predicted by equations (1) and (3). By relating the gate voltage through equation (4) to the magnetic field, this signature is seen to coincide with that of intrinsic anisotropy discussed theoretically and observed experimentally in the transport through real magnetic adatoms and molecules (27); (10); (11). The failure to close the gap at the symmetry point in Fig. 3b corresponds to a so-called ‘zero-field splitting’ (2) of such systems. During the excitation the spin transits from the lowest axial state into the planar state , see Fig. 2b. Direct transitions between the axial spin levels are spin-forbidden and do not show up in Fig. 3b. Importantly, the different energy units on the left and right -axis in Figs. 3c,d reveal that the DM-NRG gap is indeed of spintronic origin: it scales with and as predicted by equations (4)-(5) for and , respectively. We note that only for much stronger coupling the Kondo effect in Fig. 3b reinstates the characteristics similar to that in Fig. 3a. Finally, the quadrupolar gap can also be extracted from the temperature dependence of the transport quantities, see supplementary figure S-6.

Figure 4: Spin filtering. (DM-NRG) a, Linear conductance , b, average spin-quadrupole moment (normalized to its maximal value), c, linear response spin polarization of transported electrons, , shown as a function of the tunnel coupling for various values of spin polarization of the ferromagnets at the symmetry point . Solid (thin) lines correspond to the spin () quantum dot. Side diagrams (i)-(iii) illustrate schematically the competition of the energy scales of temperature (dashed lines), spintronic anisotropy (red) and Kondo spin scattering (purple), as found by DM-NRG (see Supplementary Information). Due to the -dependence, starting from thermal regime (i), first rises faster, (ii), and ultimately the Kondo effect catches up, (iii). Parameters are as in Fig. 3, except for mK, which is smaller than the temperature needed to resolve the maximally achievable gap in transport spectra of Fig. 3b (i.e. for values just before the Kondo effect sets in).

By attaching the ferromagnets we have thus obtained an artificial molecular magnet, whose quadrupolar field is strong enough to suppress the Kondo effect in a wide range of parameters, see Supplementary Information. This is expected from the analysis(28); (29); (30) of the destructive effect of intrinsic uniaxial anisotropy on the Kondo resonance (10); (11). Notably, here both these effects are generated by , cf. Fig. 4. This has important experimental implications: not only does spintronic anisotropy modify an existing, intrinsic anisotropy barrier (induced by spin-orbit interaction) (31), but it can even create such a barrier from scratch (without spin-orbit coupling), thus generating the entire observed spin-excitation spectrum. Consequently, care must be taken when using spin-polarized electrodes to search for signatures of intrinsic superparamagnetism: tunneling-renormalization effects, observed for electronic excitations (32), also affect the quantitative extraction of intrinsic anisotropy parameters, in particular when the spin polarization becomes significant, as desired in spintronics, and the tunnel coupling becomes strong. So far, the parameters were chosen to enable a comparison of the results obtained by the complementary methods used. Having established the scaling (5), we can now give a conservative estimate for the spintronic anisotropy barrier: it can be as large as 0.04 meV, i.e. the gap is clearly resolvable at mK, see Supplementary Information. This value is comparable with in the range of tens of eV for single-molecule magnets (2); (11); (14), while can reach up to few meV for some adatoms (1); (33).

Enhanced spin filtering

Finally, the spintronic quadrupolar exchange field can also be used to enhance the linear-response spin filtering of electrons transported through a quantum dot with zero dipolar exchange field and average spin. Fig. 4a presents the linear conductance (DM-NRG) as function of the tunnel coupling for fixed, intermediate temperature at the symmetry point where (see Supplementary Information). We observe that with increasing spin polarization of the ferromagnets, the value of for which the Kondo unitary conductance is reached strongly increases. This shift is caused by the spintronic anisotropy, evidenced by the finite quadrupolarization in Fig. 4b, which arises when – well before the Kondo effect sets in. Interestingly, the conductance spin polarization in Fig. 4c shows a corresponding peak that develops into a 100%-plateau for close to, yet still less than 1. But even for 50% polarized ferromagnets () the conductance spin polarization can be almost doubled if the temperature is further reduced, see supplementary figure S-8.

This amplification of the conductance spin polarization is a hallmark of the exchange quadrupolar field: in a broad, intermediate regime of -values the spintronic anisotropy gap makes the planar spin state inaccessible at low energy, as depicted in Fig. 4(ii). In consequence, tunneling induced spin-flip processes between the axial states (Kondo effect) are strongly suppressed, greatly enhancing the conductance spin polarization, see Supplementary Information. Such a behaviour is absent in the results for shown for comparison as thin curves in Fig. 4c: in this case, spin reversal does not involve a planar state.

This enhanced spin-filtering effect illustrates a promising synergy of spintronics and nanomagnetism. The spintronic anisotropy may offer new possibilities for combining tools and insights from these two research fields. As we show in Supplementary Information, one may envision to utilize the quadrupolar field as a new means for fast, electrical control of nanomagnetic memory cells, allowing even for on-demand bistability. Furthermore, in contrast to intrinsic anisotropy, the spintronic anisotropy can also be turned off magnetically by switching the spin-valve to the antiparallel configuration. Finally, it is interesting to ask whether spintronic anisotropy may be understood in a broader context: just as the dipolar exchange field term in equation (1), expressing the spin torque, can be seen as a part of the spin(-dipole) current, so, perhaps, the quadrupolar exchange field term may relate to a spin-quadrupole current (34).

Methods

The model of a high-spin quantum-dot spin valve in Fig. 1c consists of a single spin-degenerate orbital level, tunnel-coupled to two ferromagnets, and involving the local isotropic Heisenberg exchange coupling to an immobile impurity. Electron tunneling through the junctions is assumed to be symmetric and spin conserving.

Real-time diagrammatic (RTD) perturbation theory

By integrating out the ferromagnets held at different equilibria we obtain a stationary quantum kinetic equation for the reduced density operator , , where is the zero-frequency kernel expanded formally in powers of . We rewrite where is the renormalization of the Hamiltonian including both orders and which can be identified diagrammatically and then calculated. See Sec. IIA of Supplementary Information for a more detailed account. In the Coulomb blockade regime reduces to a trivial constant and is given by equation (1), where for a single electrode has the form

(6)

This was used to plot Fig. 2a. In the limit , the expression reduces to the analytic result (3), from which equation (5) follows. As mentioned in the text, one can extend the results to the case of two electrodes , with respective electrochemical potentials : replace in equation (2) and sum over . Equation (3) remains valid as long as . Finally, we recall that the dipolar exchange field in order vanishes at the symmetry point , cf. equation (4) and Fig. 2a. This also holds for irrelevant higher-order corrections in to , as the zero average spin, obtained from DM-NRG calculations at the symmetry point, demonstrates for any values of and .

Density-matrix numerical renormalization group

We use the Flexible DM-NRG (35) approach to numerically calculate the spin-resolved equilibrium spectral function [], referred to also as LDOS, of the orbital level for parallel polarization of the ferromagnets. From this we compute the spin-resolved linear-response conductance

(7)

where . Moreover, by approximating at low and low, but finite bias voltage with the symmetrized, dimensionless equilibrium spectral function , we can infer useful qualitative conclusions about the differential conductance, taking into account known limitations of this approximation. Further details can be found in Sec. IIB of Supplementary Information.

Acknowledgements.
We acknowledge stimulating discussions with J. Barnaś, A. Cornia, S. Das, J. König, S. J. van der Molen, J. Splettstoesser, I. Weymann, and H. van der Zant. The use of the SPINLAB computational facility and the open access Budapest flexible DM-NRG code (35) (http://www.phy.bme.hu/~dmnrg/) is kindly acknowledged. We acknowledge the financial support from the DFG (FOR 912), the Foundation for Polish Science (M.M.) and the Alexander von Humboldt Foundation (M.M.). Correspondence and requests for materials should be addressed to M.M.. Supplementary Information accompanies this paper on www.nature.com/naturephysics.

Author contributions

M.W. conceived the idea. M.H. and M.M. performed the analytic and numerical calculations, respectively. M.H. provided M.M. and M.W. with fitting formulas for the physical analysis of DM-NRG results. M.M. prepared the initial manuscript. All authors contributed in writing the manuscript.

Competing financial interests

The authors declare no competing financial interests.

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