Josephson Effect through an Isotropic Magnetic Molecule

Josephson Effect through an Isotropic Magnetic Molecule

Minchul Lee Centre de Physique Théorique, UMR6207, Case 907, Luminy, 13288 Marseille Cedex 9, France    Thibaut Jonckheere Centre de Physique Théorique, UMR6207, Case 907, Luminy, 13288 Marseille Cedex 9, France    Thierry Martin Centre de Physique Théorique, UMR6207, Case 907, Luminy, 13288 Marseille Cedex 9, France Université de la Méditerranée, 13288 Marseille Cedex 9, France
Abstract

We investigate the Josephson effect through a molecular quantum dot magnet connected to superconducting leads. The molecule contains a magnetic atom, whose spin is assumed to be isotropic. It is coupled to the electron spin on the dot via exchange coupling. Using the numerical renormalization group method we calculate the Andreev levels and the supercurrent and examine intertwined effect of the exchange coupling, Kondo correlation, and superconductivity on the current. Exchange coupling typically suppresses the Kondo correlation so that the system undergoes a phase transition from 0 to state as the modulus of exchange coupling increases. Antiferromagnetic coupling is found to drive exotic transitions: the reentrance to the state for a small superconducting gap and the restoration of 0 state for large antiferromagnetic exchange coupling. We suggest that the asymmetric dependence of supercurrent on the exchange coupling could be used as to detect its sign in experiments.

pacs:
73.63.-b, 74.50.+r, 72.15.Qm, 73.63.Kv

Molecular spintronics Rocha05 aims at exploring spin-dependent electronic transport through molecules with intrinsic degrees of freedom such as spin, connected to leads of various nature. On the theoretical and experimental side, recent advances have concerned both coherent Romeike1 and incoherent Elste ; Romeike2 ; Heersche06 transport through these molecular quantum dot magnets (MQDM). They consist of a magnetic molecule with either a large Sessoli93 or a small anisotropy, as is the case for a endofullerene molecule Grose .

Here, we provide a nonperturbative computation of the low temperature transport properties of a MQDM connected to superconducting leads using a numeral renormalization group (NRG) approach. The Josephson current allows a diagnosis of the interaction between the intrinsic spin of the molecule, its itinerant electron spin, and the polarization of the leads. It has been known for some time Shiba69 ; Glazman89 ; Spivak91 ; Rozhkov , and recently analyzed in experiments vanDam06 , that a quantum dot sandwiched between superconducting leads can show a junction behavior ExpPiJunction . At the same time, a quantum dot connected to leads at low enough temperatures exhibits the Kondo effect golhaber_gordon . It was shown Glazman89 ; Choi04 ; Siano04 that with superconducting leads, at low temperature the 0 junction state of the Josephson current is restored when the Kondo temperature exceeds the superconducting gap. The stability of this Kondo phase is put in question in the presence of additional spin degrees for freedom Bergeret06 which may compete with Kondo screening. Here the Josephson current flows through an isotropic MQDM which can describe a endofullerene molecule Kasumov05 . The electron spin in the quantum dot and the magnetic ion inside it interact via an exchange coupling Elste . We calculate the Andreev level (AL) spectrum and the supercurrent and determine the spin of the ground state. We find that the exchange coupling typically suppresses the Kondo effect and drives a transition from 0 to state. Moreover, antiferromagnetic coupling is found to drive exotic transitions: the reentrance to state for small superconducting gap and the restoration of 0 state for large .

The MQDM connected to two -wave superconducting leads (inset of Fig. 1) is modeled by a single-impurity Anderson model: , where

(1)
(2)
(3)

Here () destroys an electron with energy , and spin on lead (on the carbon cell); and are occupation operators for the leads and the cell. The single-particle energy can be tuned by gate voltages. denotes the exchange energy between the ion spin and the electron spin . is the superconducting gap. Except for the finite phase difference , the leads are identical and their coupling to the MQDM is symmetric. The hybridization between the molecule and the leads is well characterized by a tunneling rate , where is the density of states of the leads at the Fermi energy. As we are interested in the low temperature behavior, we concentrate for the most part on the Kondo regime with a localized level with large charging energy . Specifically, we choose (the band width is taken as a unit of energy), , and and introduce the bare Kondo temperature (at ). The energy spectrum is found with the NRG method NRG extended to superconducting leads Yoshioka00 ; Choi04 . Within the NRG method, the supercurrent is directly obtained by evaluating the expectation value of the current operator Choi04 .

Figure 1: (color online) Schematic phase diagram of a MQDM superconducting junction system [see the upper inset] indicating the 0, 0’ (blue), (green), and regions. Each region is divided into two subregions according to the ground-state spin: and for and regions and and for and regions, respectively. Note that the state exists only along the line [see the lower inset]. For larger molecular spin (see the dotted lines), the phase boundaries between and are shifted toward smaller , and one between and moves toward larger .

Fig. 1 shows the phase diagram of our system, which constitutes the main result. The junction property switches between 0 and state, depending on the strengths of and with respect to . For , the system undergoes the Kondo-driven phase transition Glazman89 ; Choi04 ; Siano04 : The ground-state wave function is of spin singlet kind for and of spin doublet for . In the strong coupling limit () Kondo correlations screen out the localized spin and Cooper pairs tunnel through the Kondo resonance state, resulting in a 0-junction Choi04 ; Siano04 . In the weak coupling limit (), strong superconductivity in the leads leaves the local spin unscreened and the tunneling of Cooper pairs subject to strong Coulomb interaction acquires an additional phase , making a -junction Shiba69 ; Glazman89 ; Spivak91 ; Choi04 ; Siano04 . It is also found Choi04 that the transition is -dependent so that a narrow region of the intermediate states and exists; see the enlarged view in Fig. 1.

Figure 2: (color online) (a) ALs in units of and (b) supercurrents in units of as functions of in the strong coupling limit () for various values of : see the line in Fig. 1. Here the ion spin is set to .

Finite exchange coupling between electron spins and the ion spin introduces another electronic correlation and affects Cooper pair transport. Fig. 2 shows typical variations of ALs and supercurrents with along the line (see Fig. 1) in the strong coupling limit (). Any finite clearly induces a splitting in subgap excitations and consequently causes a crossing between the ground state and the lowest excitation at (at least for ); the level crossing otherwise takes place only at . Across the crossing, the ground state spin is changed from to for . Similarly, the ALs defined as the one-electron/hole subgap excitations (identified as the poles of the dot Green’s functions Andreev ) exhibit discontinuities like kinks in the spectra; for two outmost ALs with spin with respect to the spin- ground state cannot remain as (spin-1/2) one-electron excitations with respect to the ground state with spin at the transition and are replaced by new ALs with spin . In parallel with an abrupt change in ALs, the supercurrent-phase relation (SPR) shows a discontinuous sign change (note that , as the continuum-excitation contribution is negligible Andreev ), culminating in a transition from 0 to state: two states labeled as are identified according to the ground-state spin , respectively. The intermediate states and are defined as in Ref. Rozhkov . The full 0 state exists only at because any small drives the system to the state at ; see Fig. 2. The curve of then has three distinct segments Choi04 . The central segment resembles that of a short ballistic junction, while the two surrounding segments are parts of -junction curve. As grows in magnitude the central segment shrinks and eventually vanishes. The SPR then becomes sinusoidal like in a tunnel junction. It should be noted that the 0- transition is asymmetric with respect to the sign of : the transition for takes place at , where is the exchange-coupling energy gap, while the 0 state survives much larger ferromagnetic coupling (). Once the -junction is fully established, stronger ferromagnetic coupling does not lead to any qualitative change in the SPR, while a second transition back to 0 state is observed for large antiferromagnetic coupling . The NRG results distinguish the second 0 state () from the former one () in three points: (1) the ground state has spin like the phase, (2) the SPR is that of a tunneling junction, and (3) the - transition has no intermediate state. Figure 3 (c) shows that the critical current has its maximum at and decreases with increasing rapidly across the phase boundary for or rather gradually for . The critical current totally vanishes at the - boundary and increases again slowly with in phase (see the curve for ).

The 0- transitions (- and -) can be attributed to the competition between superconducting and Kondo correlations as in the absence of exchange coupling. The relevant parameters are then the Kondo temperature and the superconducting gap , and the 0- phase transition occurs when they are comparable to each other: In our choice of parameters the transition happens at . The exchange coupling manifests itself by renormalizing the Kondo temperature . To see this, we applied the poor man’s scaling theory to a corresponding Kondo Hamiltonian with no superconductivity and : , where is the spin operator for the lead electrons at molecule site. The last term describing direct coupling between spins of the ion and the lead electrons arises during the scaling process. The renormalization group analysis leads to the following scaling equations: together with ,

(4)

As the band width is decreased from to , the coefficient , responsible for the Kondo correlation, diverges and the scaling breaks down. In the presence of finite exchange coupling, however, since with and , the term proportional to in Eq. (4) turns out to slow down the flow of and accordingly lowers the Kondo temperature. This point is confirmed by NRG calculations applied in the absence of superconductivity. As can be seen in Fig. 3 (a) and (b), the width of the spectral density for dot electrons, identified as the Kondo temperature , decreases with increasing (for this decrease, being marginal, is not clearly shown with the logarithmic scale). We find out that for the ferromagnetic case the ratio coincides with . For the antiferromagnetic case, the Kondo correlation is observed to be suppressed not only by the Kondo peak narrowing but by lowering the peak height.

Figure 3: (color online) Spectral weights for dot electrons coupled to normal leads with antiferromagnetic [(a)] and ferromagnetic [(b)] exchange coupling to ion spin for various values of (as annotated). (c) Critical currents as functions of for different values of (see the annotations). The arrows locate transition points corresponding to data with the same color. Here we have used .

Antiferromagnetic exchange coupling can, on the other hand, exert a more profound effect than simply renormalizing the Kondo temperature: it gives rise to a reentrant transition to the state at small and restoration of the 0 state for large . It is known that small antiferromagnetic exchange coupling , studied in the context of coupled impurities Vojta02 and side-coupled quantum dot systems SCQD and observed in experiments Roch08 , can produce a two-stage Kondo effect. After the magnetic moment of the dot is screened by conduction electrons below , at a much lower energy scale (denoted as ) the ion spin is screened by the local Fermi liquid that is formed on the dot. is then the Kondo temperature of a magnetic moment screened by electrons of a bandwidth and density of states SCQD : . The second Kondo effect leads to a Fano resonance and makes a dip in the dot electron density of states as shown in Fig. 3 (a). The dip becomes widened with and overrides the Kondo peak when so that the Kondo effect is completely overridden. As long as , the second Kondo effect does not appear since the superconducting gap blocks any quasi-particle excitation with energy less than . For , however, Cooper pairs notice the suppression of the Kondo resonance level, and their tunneling is governed by cotunneling under strong Coulomb interaction, forming a -junction again. Since decreases with decreasing , decreases to zero as . Note that the extremely small (unless ) might make it hard to detect the reentrance even under rather weak thermal fluctuations with .

The revival of the 0-state for strong antiferromagnetic coupling can be explained in the picture of cotunneling of Cooper pairs Spivak91 . In weak coupling limit, the fourth-order perturbation theory leads to the supercurrent:

(5)

where , , , and . For antiferromagnetic coupling, the ground state for the uncoupled system has spin . After one electron tunnels through the molecule the system can be in spin eigenstate of either and . The latter virtual process, costing more energy by the gap , turns out to acquire a phase, contributing to a negative supercurrent. The larger amplitude of this process by a factor (degeneracy of the spin state dominates over spin-preserving process as long as the gap is small. For a large gap , however, this process becomes negligible and the sign of the supercurrent is reversed. Note that according to Eq. (5) the SPR is always sinusoidal and the current should vanish at the transition, which is also confirmed in our NRG calculations.

Figure 4: (color online) (a) ALs in units of and (b) supercurrents in units of as functions of with and (at ) while the gate voltage is tuned from to . See the line in Fig. 1.

The physical arguments for the 0- transitions discussed so far are valid for arbitrary values of the ion spin , while the phase boundaries are shifted with changing as shown in Fig. 1. The exchange-coupling energy gap that is supposed to compete with increases with so that for larger the transitions can occur at smaller . On the other hand, we have observed that the - transition takes place at slightly larger for larger . This is because the increase in the degeneracy factor overwhelms the decrease in matrix elements due to a larger energy cost by [see Eq. (5)].

Finally, we present potential experimental manifestations of exchange-coupling-driven 0- transition. While the direct control of exchange coupling in molecules is difficult to achieve, the relative strength can be controlled by the gate voltage which can tune the Kondo temperature. Fig. 4 proposes a possibility to observe a double transition (along the line in Fig. 1) as the gate voltage is swept. Note that the double transition is an evidence of strong exchange coupling : for examples, with measured in a recent C single-molecular transistor Roch08 , one estimates . Asymmetry of the phase diagram enables the sign and possibly the amplitude of to be determined without ambiguity by observing the evolution of the SPR or the critical current.

The authors thank W. Wernsdorfer, F. Balestro, and Mahn-Soo Choi for helpful discussions. This work is supported by ANR-PNANO Contract MolSpintronics No. ANR-06-NANO-27.

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