Jan 17, 2012 - the different aspect ratios of short weak links and long ... pairs tunneling at different points of the junction width is (Fig. 1(c)): Î¸(y)=2Ï. 2e h.
Dec 18, 2007 - In a wide SNS (N being a normal metal layer) junc- tion Ic has a similar .... H = âHx is applied in the plane of N layer perpendicu- lar to the ...
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Oct 30, 2009 - of the 0 and Ï junction closely follows a Fraunhofer pattern, indicating a homogeneous ..... In the lower graphs data for the 0-Ï junction are.
Jul 30, 2013 -  J.H. Miller, Q.Y. Ying, Z.G. Zou, N.Q. Fan, J.H. Xu,. M.F. Davis ... mat/9705283).  D.F. Agterberg, M. Sigrist, A. Schnidrig, and T.M. Rice,.
May 16, 1999 - arXiv:cond-mat/9905223v1 [cond-mat.supr-con] 16 May 1999 ..... This is expected since it goes to a point in the unstable (1, 2) branch of the.
is applied to the subharmonic gap structure (SGS); simple analytical results are ... In the general case, the exact solution is found in terms of chain-fractions, and.
Jan 28, 2010 - the normal wire leads to a highly non-sinusoidal current- phase relationship, in a good agreement with Ref. . We consider a diffusive normal ...
Mar 13, 2018 - pattern) caused by real magnetic fields passing through the junction. The absence of oscillatory supercurrent originates from the fact that strain-induced gauge fields have opposite ... charged particle propagating over a path C will a
of the Hall voltage in SNS junctions has a form of narrow pulses with the Josephson ... Ïc = eH/mc is the cyclotron frequency; H is the magnetic field and eb the.
(SNS) junction are calculated for multi-mode junction with arbitrary electron ..... where Ik = (eâ2/2Â¯h)Dk sinÏ/Îµk is the contribution to the supercurrent from one of ...
Jul 28, 2013 - to finite-voltage transport properties of mesoscopic Josephson junctions with high electron transparency. ... quantitative description of MAR in junctions with arbitrary electron transparency D  is based on the usual scattering ....
The opening of these superchannels leads to a supercurrent quantization which exhibits a ... steps associated with the opening of transverse channels, ... gap in the banks). However, contrary to the universality of the quantization in a normal contac
Apr 18, 2007 - between theory an experiment, since in reality the mis- .... which accounts automatically for the normalization con- dition. ..... This means that it is reduced by approximately a factor 6, which is the same reduction factor obtained f
Jul 29, 1999 - rent as the channel is switched on and off. The supercurrent I flowing through the junction splits into the two contributions from the discrete (Idis) ...
Dec 6, 2014 - h e e. 2e. Ð. -Ð. A(E). R(E). Figure 1. Multiple Andreev reflections in ... In diffusive SNS junctions, the electron-hole coherence in the normal ...
Feb 1, 2008 - with some sâwave admixture, d + Î±s. The deviation from purely d-wave behavior ..... IV. CONCLUSION. As discussed by Sun et al. , the results of their Pb-YBCO c-axis Josephson tunneling experiments can be interpreted as showing tha
expected in superconducting tunnel and SNS junctions whose subgap conductivity ... lation numbers ne,h(E,x) of electrons and holes within the normal metal, 0 ...
Mar 16, 2010 - (Dated: November 25, 2013). We have realized multifacet Josephson junctions with periodically alternating critical current density (MJJs) using superconductor-insulator-ferromagnet-superconductor heterostructures. We show that anomalou
tors) attached to superconductors is a subject of perma- nent interest and .... the reservoirs maintain the equilibrium at the NS bound- aries, f(E, Â±d) = 2nF (E); on ...
Dec 9, 2014 - dissipative part ReY (Ï) peaks when the minigap closes (at a phase difference of Ï) even at high temperatures, when the equilibrium .... normal part ÏD and inelastic scattering rate Ïin, as was clearly demonstrated recently22. ....
It is useful to express the LDOS and the MLDOS in explicit form ...... Lett. 96 (2006), 237203.  R. Chirla, C. P. Moca, and I. Weymann, Phys. Rev. B 87 (2013) ...
Feb 1, 2008 - than the elastic mean free path le but smaller than the phase-coherence ... reflections (MAR) process leads to a sub-gap structure .... c (at. 5.5 K) demonstrates that this behavior corresponds to a low-energy excess current. The observ
Magnetic Interference Patterns and Vortices in Diffusive SNS junctions J.C. Cuevas and F.S. Bergeret
arXiv:0707.2460v1 [cond-mat.supr-con] 17 Jul 2007
Departamento de F´ısica Te´ orica de la Materia Condensada, Universidad Aut´ onoma de Madrid, 28049-Madrid, Spain (Dated: October 31, 2018) We study theoretically the electronic and transport properties of a diffusive superconductornormal metal-superconductor (SNS) junction in the presence of a perpendicular magnetic field. We show that the field dependence of the critical current crosses over from the well-known Fraunhofer pattern in wide junctions topa monotonous decay when the width of the normal wire is smaller than the magnetic length ξH = Φ0 /H, where H is the magnetic field and Φ0 the flux quantum. We demonstrate that this behavior is a direct consequence of the magnetic vortex structure appearing in the normal region and predict how such structure is manifested in the local density of states. PACS numbers: 74.45.+c,74.50.+r,74.25.Qt
Introduction.– The study of the modification of the properties of a normal metal in contact to superconductors, known as proximity effect, has a long history1 . In the last years there has been a renewed interest in this subject because new experimental techniques have allowed resolving properties on smaller length scales and very low temperatures2 . Although many electronic and transport properties of hybrid SN structures are now well understood, the situation is less satisfactory when dealing with the magnetic field dependence of those properties. A few years ago, Heida et al.3 measured the critical current as a funcion of a perpendicular magnetic field in ballistic SNS junctions of comparable length and width and found a periodicity close to 2Φ0 , where Φ0 = h/2e is the flux quantum, instead of the standard Φ0 of the Fraunhofer pattern4 . This was qualitatively explained in Refs. [5,6] in terms of the classical trajectories associated with current-carrying Andreev states in a normal clean wire. In the case of diffusive junctions, numerous experiments have shown that in wide junctions the critical current exhibits a Fraunhofer-like pattern7,8 . However, very recent experiments in junctions where the width is comparable to the superconducting coherence length have shown a monotonous decay of the critical current with field, i.e. the absence of magnetic interference patterns9 . The unified description of these two very different behaviors is a basic open problem. In this Letter we show that the solution to the previous puzzle is closely related to the issue of the formation of a magnetic vortex structure in the normal conductor. Vortex matter in mesoscopic superconductors has been also a very active subfield in superconductivity in the last years10 . It has been shown that basic properties such as critical fields11 and the magnetization12 depend crucially on the size and topology of the mesoscopic samples, which in turn determine the vortex structure. There is also a great interest in the study of nucleation of superconductivity and vortex matter in hybrid structures13 . However, little attention has been paid to the formation of vortices inside nonsuperconducting materials. Our goal here is to answer the following fundamental questions: Is it possible to induce a vortex structure in a normal wire by proximity to a superconductor?, if so, what are the properties of such proximity vortices and their influence on the Josephson effect? For this purpose, we have studied a diffusive SNS junction in the presence of a perpendicular magnetic field. By solving the two-dimensional Usadel equations14 , we are able to describe the electronic properties for arbitrary length, L, and width, W , of the normal wire. We find that a magnetic vortex structure may develope in the normal metal. These vortices have similar properties to those in the mixed state of a type II superconductor15 . The consequence of this vortex structure is the appearance of an interference p pattern in the critical current that tends to the Fraunhofer pattern in the wide-junction limit (W ≫ ξH = Φ0 /H), and also a modulation of the local density of states in the normal wire. On the contrary, when W is comparable or smaller than ξH , the formation of vortices is not favorable and the field acts as a pair-breaking mechanism which suppresses monotonously the critical current. Our results not only solve the puzzle described above, but also illustrate the richness of the vortex physics in hybrid structures. Quasiclassical formalism.– We consider a SNS junction, where N is a diffusive normal metal of length L and width W coupled to two identical superconducting reservoirs with gap ∆. The junction is subjected to an uniform external field H = H zˆ perpendicular to the normal film lying in the xy-plane, where x ∈ [0, L] and y ∈ [−W/2, W/2]. For the sake of simplicity, we assume that the thickness of the normal wire is smaller than the London penetration depth, which means that the field penetrates completely in the normal region. In order to describe the electronic properties of these junctions we use the quasiclassical theory of superconductivity in the diffusive limit14,16 , where the mean free p path is much smaller than the coherence length, ξ = ~D/∆, D being the diffusion constant of the normal metal. In equilibrium situations like the one considered here, this theory can be formulated in terms of momentum averaged ˆ R (R, ǫ), which depend on position R and energy ǫ. This propagator is a 2 × 2 matrix in retarded Green functions G
2 electron-hole space ˆR = G
GR F R F˜ R G˜R
which satisfies the stationary Usadel equation, which in the N region reads16 ~D ˆ R ˇ ˆ R ˆ R ] = ieD A[ˆ ˆ R∇ ˆ R ]. ˇG τ3 , G ∇ G ∇G + ǫ[ˆ τ3 , G π π
ˇ = ∇ˆ Here, A is the vector potential, ∇ 1 − (ie/~)Aˆ τ3 , τˆ3 is the Pauli matrix and the Coulomb gauge (∇A = 0) ˆ R )2 = −π 2 ˆ1 and proper boundary has been already used. Eq. (2) is supplemented by the normalization condition (G conditions. For the SN interfaces we use the boundary conditions introduced in Ref. , which allow us to describe the system for arbitrary transparency. For the metal-vacuum borders of the normal wire we impose that the current density in the y-direction vanishes at y = ±W/218 . In general, the Usadel equation has to be solved together with the Maxwell equation ∇ × H = µ0 j in a self-consistent manner. However, we are interested here in the case where p the width W is smaller than the Josephson penetration length λJ = ~/2µ0 ejc d, where jc is the critical current per unit area and d is the effective length of the junction including the London penetration depths in the leads. In this case one can ignore the screening of the magnetic field by the Josephson currents and the field is equal to the external one4 . The physical properties we are interested in can be conveniently expressed in terms of the Usadel-Green functions. Thus for instance, the local density of states is given by ρ(R, ǫ) = −ImG R (R,Rǫ)/π. To quantify the superconducting correlations we use the pair correlation function defined as F (R) = (1/4πi) dǫ(F R − F A ) tanh(βǫ/2), where β = 1/kB T . This function, apart from the atractive coupling constant, is the pair potential in a superconductor and it is non-zero inside the normal metal due to the proximity effect. Finally, the supercurrent density in the junction can be written as Z ∞ βǫ σN R ˜ R − F˜ R ∇F R + 4ie AF R F˜ R , Re F ∇ F (3) dǫ tanh j(R) = 4π 2 e −∞ 2 ~ where σN is the normal state conductivity. The net current is obtained integrating jx across the y-direction. Eq. (2) constitutes a set of coupled second-order nonlinear partial differential equations, whose resolution is a formidable task. In general, one has to resort to numerical methods. However, one can get analytical p insight in several limiting cases. By choosing the gauge A = −Hy x ˆ, one can identify in Eq. (2) the length ξH = Φ0 /H as the characteristic variation scale of the Green functions in the transversal direction due to the magnetic field. We consider first the case where the wire width W is smaller than ξH . In this case the Green functions do not vary considerably in the y-direction and one can average Eq. (2) over this direction leading to the one-dimensional equation ~D ˆ R ˆ R ˆ R ] = ΓH [ˆ ˆ R τˆ3 , G ˆ R ], τ3 , G ∂x G ∂x G + ǫ[ˆ τ3 G π 2π
2 2 where ΓH = De2 H is a depairing energy, which in terms of the Thouless energy, ǫT = ~D/L2 , can be written √ W /(6~) 2 as ΓH = ǫT (πΦ/ 6Φ0 ) , where Φ = HLW is the flux enclosed in the junction. These equations describe the effect of a pair-breaking mechanism, such as magnetic impurities, that has been studied extensively in Ref. . The other analytic case is the limit of a wide junction where W ≫ L, ξH . In this limit one can neglect the terms containing the derivatives with respect to the y-coordinate. The field also disappears from the equation and its only effect is to change the superconducting phase difference φ into the gauge-invariante combination γ = φ − 2π(Φ/Φ0 )y/W . With this result in mind, it is easy to anticipate, in particular, that critical current exhibits a Fraunhofer-like pattern in this limit. Discussion of the results.– We start by analyzing the local density of states (DOS) in the normal wire. In the absence of field the main feature is the presence of a minigap, ∆g 20,21,22 . This minigap is the same throughout the normal wire and for perfect transparency scales as ∆g ∼ 3.1ǫT in the limit L ≫ ξ. In Fig. 1 we show the local DOS in the middle (x = L/2) of a wire of length L = 2ξ for two different values of the width and the magnetic flux. Notice that for W = ξ (see upper panels), the local DOS is practically independent of the y-coordinate. Moreover, when the field is not very high, there is a clear minigap (see upper left panel), which closes at higher fields (see upper right panel). As one can see in the lower panels, when W ≫ L, the local DOS is strongly modulated along the y-direction. For low fields (Φ < Φ0 ), the minigap is still open throughout the wire, but for higher fields the minigap changes in a periodic fashion from its maximum value (equal to the value in the absence of field) to exactly zero at well-defined positions where the DOS is the normal state one. This situation is very similar to the mixed state of a type II superconductor, where the system becomes normal in the vortex cores.
FIG. 1: (Color online) Local density of states as a function of the energy in the middle of a wire of length L = 2ξ for two different values of the magnetic flux. The upper panels correspond to a wire width W = ξ and the lower ones to W = 50ξ. The different curves correspond to different values of the y-coordinate. We have assumed perfect transparency for the interfaces and a phase difference φ = 0. In panel (d) we have used thicker lines to highlight the curves where the DOS is equal to the normal state one.
These results are in agreement with the limiting cases discussed above. If the wire is narrow the magnetic field acts as a pair-breaking mechanism with depairing energy ΓH . It is well-known that the minigap is reduced by such 19,21 2 23 mechanisms and, in particular, it closes at a critical value ΓC H = π ǫT /2 , i.e. in our case at a critical flux √ C Φ = 3Φ0 . This explains the results for W = ξ. To understand the results for W = 50ξ, we remind that in the wide limit the magnetic field only enters in the gauge-invariant phase difference γ. It has been shown that in the absence of field the minigap decreases monotonously as the phase difference increases and it closes when the phase is equal to π 22 . Bearing this in mind, one can easily understand the results of Fig. 1(c,d). When γ = 0 the minigap is completely open reaching the value in the absence of field. However, when γ = π the minigap closes. For Φ = 2Φ0 and φ = 0, the phase γ takes the values ∓π at y/W = ±1/4, which explains why the two thick curves in panel (d) correspond to normal state DOS. The peculiar DOS suggests the presence of vortices in the normal wire. To confirm this idea, we have analyzed the pair correlation function, F (R). In Fig. 2 we show a color-coded map of the modulus of this function throughout the normal wire for the same values of L and W as in Fig. 1. All the panels show that F diminishes towards the center of the wire, which simply reflects the decay of the superconducting correlations inside the normal wire. The main difference is the modulation along the y-direction. In the case W = ξ, at low fields (see panel for Φ = Φ0 ) F is still finite everywhere, while for higher fields it can be very small in the center of the wire, but with practically no modulation. The situation changes drastically for W = 50ξ, where one can clearly see the appearance of a linear array of vortices located on x = L/2 with normal cores where F vanishes. The number of vortices depends simply on the number of flux quanta in the junction. It is important to distinguish these vortices from the so-called Josephson vortices that take place in much wider junctions where W > λJ and the self-field effects play a crucial role4 . An important difference is that the Josephson vortices do not have normal cores and their size is comparable to λJ . It is possible to get an analytical insight into the vortex structure by using the linearized Usadel equations in the wide-junction limit. In this case one can show that the position of the zeros of the pair correlation function are given
FIG. 2: (Color online) Spatial map of the modulus of the pair correlations, |F (R)|, for L = 2ξ and φ = 0. The different panels correspond to different values of the width W and the magnetic flux Φ, as indicated in the graphs. |F (R)| has been normalized to its value inside the electrodes, the temperature is kB T = 0.01∆ and perfect transparency was assumed.
by L x= and φ − 2π 2
y = (2m + 1)π, W
where m = 0, ±1, ... and y ∈ [−W/2, W/2]. This means that the vortex cores are located exactly on the middle of the wire forming a regular linear array along the y-direction and they are separated by a distance Φ0 /HL. Thus, for the case W = 50ξ in Fig. 2 this condition tells us that for Φ = 4Φ0 there are four vortex cores located on y/W = ±1/8, ±3/8, which are the positions that one can read off from Fig. 2. Notice also that according to Eq. (5) the phase φ simply shifts rigidly the line of vortices along the y-direction. Thus, measurements of the local DOS at the outer interfaces (y = ±W/2) changing the supercurrent through the junction should show an oscillatory behaviour. On the other hand, the normal cores are surrounded by circulating currents (not shown here), which vanish exactly at the cores. Moreover, from the analytical solution of the linearized Usadel equation in the wide-junction limit and from the numerical results for arbitrary cases, one can easily show that the phase of the pair correlation changes in 2π around the cores, i.e each vortex has a unit topological charge. In short, the main difference with the usual
W = 0.5ξ W=ξ W = 2ξ W = 3ξ W = 5ξ W = 10ξ W = 200ξ Fraunhofer
1 W = 0.5ξ averaged result
0.6 0.2 0
0 0.5 1 1.5 2 2.5 3 3.5 4
FIG. 3: (Color online) Critical current normalized by the zero-field value vs. magnetic flux for a wire length L = 8ξ, perfect transparent interfaces and kB T = 0.01∆. The different curves correspond to different values of the width of the wire, W . The dashed line shows the standard Fraunhofer pattern given by sin(πΦ/Φ0 )/(πΦ/Φ0 ). The inset shows for W = 0.5ξ the comparison between the exact result and the approximation of Eq. (4) for the narrow-junction limit.
vortices in a bulk superconductor of type II is that they are arranged in one-dimensional array instead of forming a two-dimensional lattice and due to the confining geometry they do not possess a rotational symmetry15 . We discuss finally the magnetic field dependence of the critical current. In Fig. 3 we show an example for L = 8ξ, which is a typical value in the experiments9 , and different values of W . Notice that for small values of W , the critical current decays monotonously. This is simply due to the fact that in this limit no vortices appear and the field suppresses progressively the superconductivity in the normal wire19 . Indeed, as we show in the inset of Fig. 3, in this limit Eq. (4) describes quantitatively the field dependence. As the width increases the vortex structure discussed above appears and as a consequence one observes the appearance of an interference pattern where the critical current vanishes at certain values of the magnetic flux. Notice that these values are clearly larger than Φ0 for intermediate widths and the patterns are not “periodic”. Only in the limit W ≫ ξH , L one obtains a regular pattern with zeros at multiples of Φ0 , recovering the Fraunhofer pattern4 . These results explained in an unified manner the different behaviours observed experimentally7,8,9 , which at first glance seemed to be contradictory. Finally, we have studied systematically the role of the length L in the crossover from the narrow-junction to the wide-junction behavior. We have found that as L increases this transition occurs at larger values of W . This confirms the fact that the condition for the appearence of an interference pattern, i.e. zeros in the critical current, is given, roughly speaking, by W > ξH , which is equivalent to W/L > Φ0 /Φ. The standard Fraunhofer pattern is approach when W & L. Conclusions.– We have studied a diffusive SNS junction in the presence of a perpendicular magnetic field. We have shown that the appearance of magnetic interference patterns in the critical current is intimately linked to the formation of a vortex array in the normal wire. Our results provide an unified description of the critical current for arbiratry width of the junctions and solve the puzzle put forward by recent experiments9 . Our work also paves the way to study the vortex matter in a great variety of hybrid structures like the recently introduced superconducting graphene junctions, where a standard Fraunhofer pattern has been observed24 . We would like to thank Sophie Gu´eron and H´el`ene Bouchiat for numerous discussions about their experiments which motivated this work. It is also a pleasure to acknowledge useful discussions with Philippe Joyez, Hugues Pothier,
6 T.M. Klapwijk, S. Russo, A.F. Morpurgo and J.G. Rodrigo. This work has been financed by the Spanish CYCIT (contract FIS2005-06255). F.S.B. acknowledges funding by the Ram´ on y Cajal program.
2 3 4 5 6 7 8
11 12 13 14 15
19 20 21 22 23 24
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