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Incoherence and enhanced magnetic quantum oscillations in the mixed state of a layered orga_图文

arXiv:cond-mat/0502462v1 [cond-mat.supr-con] 18 Feb 2005

Incoherence and enhanced magnetic quantum oscillations in the mixed state of a layered organic superconductor
V. M. Gvozdikov1,2 and J. Wosnitza3[*] 1Max-Planck-Institut fu¨r Physik komplexer Systeme, D-01187 Dresden, Germany
2Kharkov National University, 61077, Kharkov, Ukraine 3Institut fu¨r Festk¨orperphysik, Technische Universit¨at Dresden, D-01062 Dresden, Germany
(Dated: February 2, 2008)
We present a theory which is able to explain enhanced magnetic quantum-oscillation amplitudes in the superconducting state of a layered metal with incoherent electronic transport across the layers. The incoherence acts through the deformation of the layer-stacking factor which becomes complex and decreases the total scattering rate in the mixed state. This novel mechanism can compensate the usual decrease of the Dingle factor below the upper critical magnetic ?eld caused by the intralayer scattering.
PACS numbers: 71.18.+y, 72.15.Gd, 74.70.Kn

In recent years it has been questioned whether the electronic properties of layered quasi-two-dimensional (2D) metals can be described within the usual fundamental concept of an anisotropic three-dimensional Fermi liquid [1]. Well-studied examples, besides the cuprate superconductors and quasi-one-dimensional organic metals, are organic conductors of the type (BEDT-TTF)2X, where BEDT-TTF stands for bisethylenedithio-tetrathiafulvalene and X for a monovalent anion. This class of materials displays a number of unique properties such as an unconventional electronic interlayer transport, clear deviations of their magnetic quantum oscillations [2] from the standard three-dimensional (3D) Lifshitz–Kosevich theory [3], and puzzling features in the superconducting mixed state. After the ?rst observation of the de Haas– van Alphen (dHvA) oscillations in the mixed state of a layered superconductor [4] it was ?rmly established that these oscillations are damped below the upper critical ?eld Bc2. This damping was explained by several mechanisms reviewed in [5]. A recent observation that both the dHvA and the Shubnikov–de Haas (SdH) amplitudes are enhanced in the mixed state of the layered organic superconductor β′′-(BEDT-TTF)2SF5CH2CF2SO3 (β′′ salt in the following) [6] was a real surprise since it is in sharp contrast to all experiments and theories known so far [5].
Theoretically, it is assumed that the quasiparticle scattering by the “vortex matter” just below the upper critical ?eld, Bc2, is the main mechanism of the damping in this region yielding the Dingle-like additional damping factor Rs = exp(?2π/?τs). Here, ? is the cyclotron frequency and /τs is the sum of the two terms
/τs1 = ?2(π/? ?)1/2, due to the intralayer scattering at vortices [7, 8, 9], and /τs2 = β?2/??τ0, which takes into account the scattering by impurities and vortices within the layers [10]. (τs is the scattering time, ? is the chemical potential, ? is the superconducting order parameter which just below Bc2 is less than the Landaulevel separation ? < ?, and β ? 1.)
The additional factor Rs describes the extra damp-

ing of the dHvA and SdH amplitudes only due to the intralayer scattering in 2D conductors. Within this concept, however, the oscillation-amplitude enhancement in the β′′ salt is not explicable. Anomalous dHvA oscillations have also been observed in YNi2B2C [11, 12]. These oscillations persist down to the surprisingly low ?eld 0.2Bc2 [12]. A Landau-quantization scheme for ?elds well below Bc2 in the periodic vortex-lattice state was developed in [13] and for a model with an exponential decrease of the pairing matrix elements in [10]. The observed recovery of the dHvA amplitudes for B ? Bc2 in YNi2B2C was explained by the enhancement of the special vortex-lattice factor depending on the Landau bands which become narrower when the vortex-lattice grows thinner [10].
The anomalous magnetic quantum oscillations in the mixed state of the β′′ salt is much more mysterious and poses the question on the peculiarity of this material. The β′′ salt is the only among the known superconductors which (i) displays enhanced magnetic quantumoscillation amplitudes in the mixed state and (ii) has no 3D Fermi surface (FS), i.e., exhibits an incoherent electronic transport across the layers [14]. The incoherence means that the electronic properties of this layered quasi-2D metal cannot be described within the usual fundamental concept of an anisotropic 3D FS. Nonetheless, magnetic oscillations due to the 2D FS survive [1].
Here, we consider a new mechanism for the quasiparticle scattering that goes beyond the usual 2D consideration of intralayer scattering by taking into account the interlayer-hopping contribution to the total scattering rate. This can explain an oscillation-amplitude enhancement in the superconducting state for layered conductors with incoherent hopping across the layers. The clear physical picture behind this mechanism is as follows. The incoherence, or disorder in the direction perpendicular to the layers, hampers the electron hopping between neighboring layers. This enhances the scattering at impurities within the layers since electrons on a Lan-

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dau orbit interact with the same impurities many times before a hopping to the neighboring layer occurs. In the superconducting state long-range order establishes across the layers which allows quasiparticles to escape the intralayer multiple scattering by Josephson tunneling between the layers. This mechanism reduces the scattering rate by impurities and enhances the Dingle factor in the superconducting state. For the β′′ salt this e?ect most likely plays the dominant role. For the coherent case, there is no interlayer scattering and the electrons (quasiparticles) can move freely across the layers both in the normal and the superconducting state which render the above mechanism much less e?ective. Numerically, the e?ect is described by the layer-stacking factor [Eq. (3)] which itself contains a Dingle-like exponent in the case of incoherent interlayer hopping [15]. Superconductivity restores the coherence across the layers by renormalizing the hopping integrals [16]. This reduces the interlayer scattering and enhances the oscillation amplitudes.
In case the momentum across the layers is not preserved, the electron interlayer hopping maybe described in terms of an energy ε that is distributed with the density of states (DOS) g(ε). The energy spectrum of a layered conductor in a perpendicular magnetic ?eld is, therefore, given by En(ε) = ?(n + 1/2) + ε [15]. The total DOS then follows from the standard Green-function de?nition

N (E) =

1 2π2l2

Im



n=0



E

?

En

g(ε) ?ε?

Σn(E)

,

(1)

where Σn(E) is the average self energy corresponding to the nth Landau level and l = ( e/cB)1/2 is the magnetic length. For large energies and large n ≈ E/ ? ? 1 (relevant for the magnetic quantum oscillations here) the self energy is independent on the index n and the summation in Eq. (1) by use of Poisson’s formula yields

N (E) N (0)

=

1

+


2Re (?1)pRD(p, E)Ip
p=1

exp

2πipE ?

,

(2)

where N (0) is the 2D electron-gas DOS and the func-

tion RD(p, E) = exp (?2πp|ImΣ(E)|/ ?) generalizes the

Dingle factor to the case of an energy-dependent self en-

ergy Σ(E). The layer-stacking factor in Eq. (2),

Ip =

dεg(ε) exp

2πipε ?

,

(3)

is an important factor in the theory of magnetic quantum oscillations in normal and superconducting layered systems [10, 17]. It describes contributions to the oscillations coming from the interlayer hopping. If the stacking is irregular Ip becomes complex and contains a Dinglelike exponent [15].
The inverse scattering time 1/τ (E) = |ImΣ(E)|/ in the self-consistent Born approximation (SCBA) was

found to be proportional to the total DOS [18, 19, 20]. Accordingly, the relation N (E)/N (0) = τ0/τ (E) holds, where τ0 is the intralayer scattering time [21, 22]. Substituting this into Eq. (2) leads to an equation for τ (E) showing that it oscillates as a function of 1/B.
In case the highly anisotropic electronic system has a 3D Fermi surface the DOS related to the interlayer hopping is symmetric, g(ε) = g(?ε), and becomes for nearest-neighbor hopping g(ε) = π?1(4t2 ? ε2)?1/2. The corresponding layer-stacking factor then is given by Ip = J0(4πtp/ ?). This Bessel function oscillates as a function of 1/B which is just another way to describe the wellknown bottle-neck and belly oscillations of a corrugated 3D FS. Oscillating corrections to the Ginzburg–Landau expansion coe?cients caused by the factor J0(4πtp/ ?) were also calculated in [23].
For the incoherent case, on the other hand, the translation invariance across the layers is lost. The irregular interlayer hopping means that the DOS deviates from the function g(ε) = π?1(4t2 ? ε2)?1/2 and loses the symmetry g(ε) = g(?ε) which implies that ImIp = 0. As will be shown below, this results in a special contribution to the electron scattering time. Below Bc2, this may lead to a suppression of the scattering rate acting against the known intralayer damping mechanisms of the quantum oscillations in the mixed state [5]. However, this contribution vanishes if the hopping between the layers preserves the interlayer momentum leading to a corrugated 3D FS cylinder. This is an important point in our consideration.
Using Eq. (2) and N (E)/N (0) = τ0/τ (E) we write τ (E)?1 as a sum of the coherent (symmetric) and incoherent (asymmetric) terms:

τ (E)?1 = τ (E)?s 1 ? τ (E)?a 1,

(4)

τ0 τs

=


1 + 2 (?1)pRD(p, E)ReIp cos
p=1

2πpE ?

,

(5)

τ0 τa


= 2 (?1)pRD(p, E)ImIp sin
p=1

2πpE ?

.

(6)

With the help of the summation rule



S(λ, δ) =

(?1)pe?|p|λ cos pδ =

sinh λ

(7)

p=?∞

cosh λ + cos δ

one can rewrite Eqs. (5) and (6) in the integral form

11

τs(a) = τ0 dεgs(a)(ε)S[λ, δ(E, ε)].

(8)

Here gs(ε) = gs(?ε) is the symmetric and ga(ε) = ?ga(?ε) is the antisymmetric part of the DOS g(ε),

3

λ(E) = 2π/?τ , and δ(E, ε) = 2π(E ?ε)/ ?. The SCBA, as well as Eqs. (4)-(8), are valid not only for point-like impurities but also for a smooth random potential provided its correlation radius is less than the Larmor radius, which holds for large n [20]. One can see from Eqs. (4)-(8) that, in general, the incoherent contribution, ?τ (E)?a 1, to the total scattering rate, τ (E)?1, is essential. The integral equation for τ (E)?1 is very complex and can be solved only perturbatively in the case λ ? 1. In the limit λ → ∞, when S(λ, δ) → 1, we have τs?1 = τ0?1 and τa?1 = 0. For ?nite, but large λ the parameter RD(p, E) = e?pλ ? 1. Even if ?τ ? 1, the quantity e?λ ? 1 and Eqs. (5) and (6) are just a series expansion in powers of the small parameter e?λ. Eq. (7) shows the convergence of this series for any λ > 0 allowing a perturbative solution. The perturbative terms oscillate as a function of E and can be written as the series τ ?1(E) = τ0?1[1 + X1 + X2 + O(e?3λ0 )], with X1 ∝ e?λ0 , X2 ∝ e?2λ0 , and λ0 = 2π/?τ0. The ?rst nonzero correction averaged over an oscillation period is proportional to X1 + X2 = ?2λ0e?2λ0 |I1|2 and yields

1= 1 τ? τ0

1

?

4π ?τ0

(RD0 )2

ReI12 + ImI12

.

(9)

The Dingle factor RD0 = exp (?2π/?τ0) is a small parameter in our perturbative solution. The term ImI12 in Eq. (9) appears due to the incoherence.
It was established that in the β′′ salt electron hopping across the layers is most probably incoherent, i.e., the momentum perpendicular to the layers is not preserved and there is no 3D Fermi surface [14]. The reason for this remarkable feature is unknown so far. It might be that some kind of disorder, such as di?erent spatial con?gurations in the extraordinary large and complex anionmolecule layer may induce random hopping integrals, in analogy with intercalated layered compounds [15]. Furthermore, the β′′ salt is the only material so far studied (not only among the BEDT-TTF salts) which displays an enhancement of the magnetic quantum-oscillation amplitude in the superconducting state [6].
This important result is summarized in Fig. 1. In this Dingle plot for a 2D metal the amplitudes A1 of the fundamental dHvA frequency (F ≈ 198 T) and A2 of the second harmonic (2F ) are normalized by B sinh(X)T ?1 and plotted on a logarithmic scale as a function of 1/B, with X = 2π2kBmcT /e B and mc the e?ective cyclotron mass (see [6] for more details). Upon entering the superconducting state the oscillation amplitude A1 is enhanced compared to the normal-state dependence (solid lines). For the second harmonic A2 neither an additional damping nor an enhancement is observed [24].
In the superconducting state long-range order across the layers evolves through the renormalization of the hopping integrals [16]. This can be understood as follows. The quasiparticle hopping between the layers is an independent degree of freedom with respect to the

Ai B sinh(X)/T (arb. units)

104

A1

A2 103

102

β’’-(BEDT-TTF)2SF5CH2CF2SO3
T (K) 0.03 0.12 0.35 0.54

101

100 0

0.1

0.2

0.3

0.4

0.5

0.6

0.7

1/B (T-1)

FIG. 1: Dingle plot of the fundamental (A1) and the second harmonic (A2) dHvA amplitudes of the β′′ salt extracted from modulation-?eld data for di?erent temperatures. The solid lines are ?ts to the data above 6 T.

in-plane Landau quantization. In the normal state the Green-function equation related to the interlayer hopping is given by

[(ε ? εi)δim ? tim]G0ij (ε) = δij ,
m

(10)

where the electron energy in the layer εi and the hopping integrals tim = ti(δi,m+1 +δi,m?1) are assumed to depend on the layer indices for the sake of generality. In the superconducting state the order parameters in the layers, ?i, become nonzero and the Gor’kov equation for the Green functions Gij can be written as [16]

[(ε ? εi)δim ? t?im]Gij (ε) = δij ,

(11)

m

t?im = tim ? ?iG0im(?ε)??m.

(12)

The star means the complex conjugate. When comparing Eq. (10) with Eq. (11) it is seen that in the superconducting state the e?ective hopping integrals, given by Eq. (12), become nonzero not only for next-nearest-neighbor hopping. In that case the nonvanishing retarded Greenfunction components G0im(?ε) result in nonzero t?im for electron hopping between arbitrary sites i and m. In fact, Eq. (12) simply re?ects how the superconducting long-range order establishes across the layers. The complex order parameters in the layers ?i = |?i| exp (i?) appear and result in interlayer (intrinsic) Josephson coupling [16]. In the absence of Josephson currents the order parameter can be chosen to be real and independent of the layer index ?i = |?i|. The correction to the DOS due to this mechanism is

δg(ε) = ??2

ij

?g(ε) ?tij

G0ij

(?ε).

(13)

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The second e?ect we have to take into account is caused by the vortex matter in the mixed state. Here, the vortices are disordered for ?elds slightly below Bc2. They convert the degenerated Landau levels into asymmetric Landau bands as was shown in Refs. [25, 26]. Thus, in the mixed state the quasiparticle tunneling between the layers implies the quantum transition between these Landau-band states which results in the additional contribution to the simple nearest-neighbor DOS

δg?(ε) = ?2

?g(ε)

??2

.
?=0

(14)

The total correction to the DOS in the mixed state can be written as δgtot(ε) = ?2G(ε), where G(ε) is directly de?ned by Eqs. (13) and (14). Inserting δgtot(ε) into Eq. (8) and averaging over a period in E results in

δ

1 τ

=

?2 τ0

dεG(ε)S(λ, δ(E, ?ε))

=

?2 τ0

γ.

(15)

Since the DOS is normalized ( dεg(ε) = 1) the function

G(ε) satis?es the condition dεG(ε) = 0. This means

that it is alternating in sign and γ might be negative

because S(λ, δ(E, ?ε)) > 0. The studied system is too

complex to calculate γ in general. In the limit λ → ∞

this coe?cient vanishes since S(λ, δ(E, ?ε)) → 1. It is

instructive to consider a correction to the scattering rate

in Eq. (9) in the mixed state. The variation of the layer-

stacking factor δI1 is given by Eq. (3) with the DOS replaced by δgtot(ε). The broadening of the Landau levels, caused by δgtot(ε), is of the order of the width of this function and much less then ? in order to observe the

oscillations. Therefore, in ?rst approximation ReδI1 ≈ 0

and ImδI1 = ?2

dεG(ε)

sin(

2πε ?

)



?2

(

2π<ε> ?

),

where

ε = dεG(ε)ε. (For G(ε) = ?G(?ε), ReδI1 is zero ex-

actly.) Thus, the correction to the scattering rate in the

mixed state near Bc2, caused by the interlayer-hopping mechanism, is given by

δ

1 τ?

= ??2 2ImI1 τ0

4π ?τ0

(RD0 )2

2π ε ?

.

(16)

For ε ImI1 > 0, this gives a decrease in the scattering rate. Note that the latter is nonzero only if the system is incoherent in the normal state and ImI1 = 0. This strongly supports the relevance of this mechanism for the β′′ salt, since only this organic metal displays both incoherence in the normal state and an enhancement of the SdH and dHvA amplitudes in the mixed state.
Thus, the overall e?ect superconductivity has on Rs is determined by the balance between positive and negative contributions to the scattering rate. The already mentioned positive contribution from the intralayer scattering at vortices and defects is

= ?2

π

1/2
+

β

.

(17)

τs

??

??τ0

The new additional interlayer mechanism we discuss here

results in a negative contribution given by δ

1 τ

=

?2 τ0

γ

[Eq.(15)]. Since little is known about the DOS of the

studied system, even in the normal state, we cannot cal-

culate the coe?cient γ quantitatively. However, contrary

to Eq. (17), for this term the small factor 1/? is absent,

so that the overall correction to the scattering rate might

be negative. The experimental facts [6] give us con?dence that this is the case at least for the β′′ salt.

We conclude with a qualitative picture of the e?ect
discussed here. The incoherence means that the hopping time between the layers τz ≈ /|t| ? τ0 so that an electron scatters many times within a layer before leaving it [1]. Here the quantity |t| is some averaged hopping integral that in the β′′ salt may be assumed to be the smallest parameter in energy. Indeed, experimentally |t| cannot be resolved in the β′′ salt re?ecting the fact that
the hopping integral is one of the smallest for all known
2D organic metals so far [14]. Consequently, even small
spatial ?uctuations of the hopping probability within and
across the layers render the electron motion across the
layers incoherent. On the other hand, for the evolution of
superconductivity some interlayer (Josephson) coupling
is vitally important. Long-range order establishes below
Bc2, thereby renormalizing the hopping integral. According to Eq. (12), the renormalized τz in the superconducting state may be estimated as τz ≈ /|t + ?2/t|. For ? ? |t| the hopping time reduces considerably and becomes τz ≈ |t|/?2. The latter means that the quasiparticles spend less time within the (impurity-containing)
layers decreasing the scattering rate and, consequently, enhancing the Dingle factor. In the β′′ salt this e?ect is strong because of the smallness of |t|. Thus, our mechanism relates the two unusual e?ects observed in the β′′
salt: the incoherent interlayer hopping transport and the
enhancement in the quantum-oscillation amplitudes in
the mixed state.

This work was supported in part by INTAS, project INTAS-01-0791, and the NATO Collaborative Linkage Grant No. 977292. V.M.G. thanks P. Fulde and S. Flach for the hospitality at the MPIPKS in Dresden.

[*] present address: Forschungszentrum Rossendorf, Hochfeld-Magnetlabor Dresden (HLD), 01314 Dresden, Germany
[1] R.H. McKenzie and P. Moses, Phys. Rev. Lett. 81, 4492 (1998); P. Moses and R.H. McKenzie, Phys. Rev. B 60, 7998 (1999).
[2] J. Wosnitza, Fermi Surfaces of Low-Dimensional Organic Metals and Superconductors (Springer, Berlin 1996); J. Singleton, Rep. Prog. Phys. 63, 1111 (2000).
[3] I.M. Lifshitz and A.M. Kosevich, Zh. Eksp. Teor. Fiz. 29, 730 (1956).
[4] J.E. Graebner and M. Robbins, Phys. Rev. Lett. 36, 422

5

(1976). [5] T. Maniv, V. Zhuravlev, I. Vagner, and P. Wyder, Rev.
Mod. Phys. 73, 867 (2001). [6] J. Wosnitza et al., Phys. Rev. B 67, 060504(R) (2003). [7] K. Maki, Phys. Rev. B 44, 2861 (1991). [8] M.J. Stephen, Phys. Rev. B 45, 5481 (1992). [9] A. Wasserman and M. Springford, Physica B 194-196,
1801 (1994). [10] V.M. Gvozdikov and M.V. Gvozdikova, Phys. Rev. B 58,
8716 (1998). [11] G. Goll et al., Phys. Rev. B 53, 8871 (1996). [12] T. Terashima et al., Phys. Rev. B 56, 5120 (1997). [13] L.P. Gorkov and J.R. Schrie?er, Phys. Rev. Lett. 80,
3360 (1998). [14] J. Wosnitza et al., Phys. Rev. B 65, 180506(R) (2002). [15] V. M. Gvozdikov, Sov. Phys. Solid State 26, 1560 (1984). [16] V.M. Gvozdikov, Sov. J. Low Temp. Phys. 14, 7 (1988). [17] V.M. Gvozdikov et al., Phys. Rev. B 70, 085113 (2004);
Phys. Rev. B 65, 165102 (2002); Low Temp. Phys. 27,

704 (2001). [18] T. Ando and Y. Uemura, J. Phys. Soc. Jpn. 36, 959
(1974). [19] T. Maniv and I.D. Vagner, Phys. Rev. B 38, 6301 (1988). [20] M.E. Raikh and T.V. Shahbazyan, Phys. Rev. B 47, 1522
(1993). [21] P.D. Grigoriev, Phys. Rev. B 67, 144401 (2003). [22] T. Champel and V.P. Mineev, Phys. Rev. B 66, 195111
(2002). [23] T. Champel and V.P. Mineev V. P., Phil. Mag. B 81, 55
(2001). [24] A di?erent behavior of A2 in the mixed state is not sur-
prising since for 2D metals, and especially for the β′′ salt, A2 behaves unusual even in the normal state. [25] M.R. Norman and A.H. MacDonald, Phys. Rev. B 54, 4239 (1996). [26] Z. Tesanovich and P.D. Sacramento, Phys. Rev. Lett. 80, 1521 (1998).