The rapidly extending realm of high-Tc superconductors has been enriched recently by a new class of materials, so called iron based superconductors (FeSC)1,2,3,4,5. Like many other high-Tc materials, these compounds crystallize in strongly anisotropic lattices: one can identify quasi-two-dimensional subsystems which contain the electrons that are subject to Cooper pairing. In FeSCs these planes consist of square pyramids with alternatively oriented apex vertices that are occupied by pnictogen ions and a square base formed by iron ions. A specific feature of the electronic structure of FeSC is the multipocket Fermi surface, mostly semi-metallic (with both hole and electron pockets), although some superconducting materials possess either only electron6,7 or only hole pockets8. Another characteristic feature of FeSC is the interplay between different electronic instabilities of the pristine normal metal phases. Most of these materials are unstable against spin-density wave (SDW) type itinerant antiferromagnetism, and the phase diagrams of doped compounds contains domains of superconductor (SC) and SDW ordering, the latter sometimes being accompanied by structural phase transitions with a potential for orbital ordering9,10,11,12. This means that any consistent theory of superconductivity should take into account the strong interplay between electronic and magnetic instabilities in presence of trends to orbital ordering and soft lattice displacement modes (see another more complex approach for description of d-electrons in iron pnictides in ref. 13). Such a more general approach to consider not simply a single instability of a “normal state” phase with respect to superconductivity but instead to treat on equal footing the competition (including also their coexistence) of various orderings is a generic problem for many non-standard superconductors and related phases14,15. Even the standard case of strong electron-phonon interaction mediated SC and a Fermi surface derived instability requires strictly speaking the account of possible lattice instabilities and of the related anharmonicities reducing the strength of the former. For the sake of simplicity here we will only focus on the interplay of a specific SDW and SC - a generalization to the case of higher multi-component instabilities is straightforward.

A specific motivation to consider and develop a multi-mode theory is provided by the experimental observation that in FeSCs electron or hole doping of pristine magnetic materials is crucial for suppression of itinerant SDW magnetism and formation of superconducting state. Apart from that, doping by isovalent impurities or a noticeable concentration of intrinsic defects (vacancies) can also strongly modify their phase diagram. It was noticed in this context that conventional understanding of the role of non-magnetic and magnetic impurities in formation of Cooper pairs in BCS superconductors formulated in classical papers by A.A. Abrikosov, L.P. Gor’kov and P.W. Anderson (see, e.g. refs 16 and 17) should be revisited and modified for these multiband superconductors because interband coupling plays crucial role in formation of superconducting order in these nearly nested, quasi 2D materials. Both nonmagnetic and magnetic scattering essentially influence Tc - in particular, interband scattering due to non-magnetic impurities is destructive for s± superconductivity, which is considered to be realized in most of FeSC18,19,20,21,22 and magnetic interband scattering on the contrary stabilizes the s± coupling mechanism18,23. The kinematics of this stabilization mechanism is similar to that in so called π-junctions in heterostructures superconductor/insulator/superconductor, where the Josephson tunnelling through a barrier with paramagnetic impurities is accompanied with the sign change of the superconducting order parameter Δ24. Another remarkable response to doping occurs when nominally nonmagnetic defects such as As vacancies25,26,27 or Ru substitutions28 are introduced in 1111 materials. These impurities trigger a strong paramagnetic response (see ref. 29 for explanation of this effect), and their observed modification of Tc does not fit with available theories.

To this end we introduce and develop a multi-mode theory that takes into account the fact that the superconductivity in these materials arises as a result of competition of at least two coupling mechanisms: superconducting pairing with the scalar order parameter Δ and the spin density wave ordering with vector order parameter m (the magnetic moment). These modes are coupled by the interband electron-electron interaction, and we consider the effect of impurity scattering on this coupling mechanism.

The paper is written as follows. We start with the derivation of a system of Bethe-Salpeter (BS) equations containing coupled SDW and Cooper channels for temperatures above the magnetic and superconducting transition temperatures in the next section. Based on BS equations we show that dynamical fluctuations play an important role close to the tetracritical point and must be taken into account for the correct description of the tetracritical region.

Furthermore we derive the Landau-Ginzburg (LG) functional and calculate fluctuation corrections to the phase transition temperatures to superconductor and SDW phases (Tc and Ts, respectively). Detailed derivation of BS and LG equations is given in the Section “Methods”.

Where needed, we will be specific and concentrate on the multi-valley semi-metallic FeSCs from the 1111 (ReFeAsO) and 122 (AeFe2As2) families under electron and hole doping (Re and Ae stay for the rare-earth and alkaline-earth elements) respectively.

Multimode approach to SDW and BCS instabilities

In this Section we formulate a mode coupling approach for multiband ferropnictide superconductors with nearly nested hole and electron pockets of Fermi surface. Although a complete consensus is lacking on the type of superconductor pairing in these system, it appears that the experimental arguments in favor of s± mechanism are rather solid. This type of ordering was proposed originally for superconductor-excitonic instability in semimetals30 and has been reformulated for superconductor pairing in FeSCs in refs 31, 32 (for a review see ref. 5). It is important to note that mode-mode coupling is an inherent constituent of s± pairing33,34,35: in the two-dimensional systems with nesting conditions between electron and hole pockets an interplay between the SDW and Cooper modes results in additional coupling within each channel induced by all other channels. This theory is based on a renormalization group (RG) approach, which implies logarithmic renormalization of the relevant vertices. It was shown that the Cooper and SDW decouple at the scale of Fermi energy and further flow goes independently in both channels. The natural limitation of such approach is the demand of perfect nesting in SDW channel. In real FeSC systems the nesting conditions are satisfied only approximately. It leads to the suppression of the SDW channel at some energy.

The general approach to deal with mode-mode coupling that we introduce here is based on the mode coupling theory of critical phenomena. We start from the “high temperature” region, where the critical fluctuations are already well developed, while long-range SC and SDW order are not yet established. The corresponding vertex parts Γsc(q, Ω, T) and Γsdw(Q + q, Ω, T), are represented at this temperature by the fluctuating modes Dsc(q, Ω) and Dsdw(q, Ω) respectively36,37:

with critical parameters

and γsc/sdw = 8T/π. Here we consider the limit of small momenta cΔ/mq2 1, ν is a density of states at the Fermi level, and are superconducting and magnetic coherence lengths respectively, see Section “Ginzburg-Landau approach”.

As the pole iΩsc/sdw = γsc/sdw(τc/s + cΔ/mq2) of the vertex part Γsc or Γsdw at q → 0 tends to zero, the corresponding instability results in the phase transition. When approaching the transition temperature Tc or Ts, the corresponding vertex part diverges in the static limit:

The mode coupling approach is valid in the vicinity of the tetracritical point on the phase diagram shown in Fig. 1 where the two temperatures Tc and Ts are comparable. Then the system of equations for the vertex parts at small Ω and q can be derived and solved. These are the Bethe-Salpeter equations for the most relevant vertices. As will be shown below, this system contains at least four bare vertices which should be taken into account. The divergences (3) provide us with a criterion of selecting the corresponding diagrams. Namely, the terms containing polarization operators in the electron-hole channel with transmitted momentum close to Q, and the electron-electron polarization operators of Cooper type should be collected in all orders. As a result, the system of Bethe - Salpeter equations acquires a parquet-like structure, and the solution of the mode-coupling equations obtained at T > Tc may be mapped on the mean-field solutions of renomalization group (RG) equations below Tc33,34.

Figure 1
figure 1

Phase diagram of competing SDW and SC states as a function of the carrier concentration.

The shaded area denotes the coexistence region of s± superconductivity and the SDW. The critical temperatures of SDW and SC transitions coincide in the tetracritical point. The insert shows zoomed in part of the phase diagram around the mean-field tetracritical point: the new tetracritical point (filled circle) is shifted due to fluctuations computed in the multi-mode coupling theory (dashed lines).

We assume that the superconducting transition temperature Tc is imposed on the system by a dominant s± pairing. In this Ansatz the interband electron-hole Coulomb interaction is the main source of Cooper pairing, so that a weak BCS attractive interaction in the electron and hole pockets would result in SC instabilities with .

Bethe-Salpeter equations

Following the Ansatz formulated above (see details in the Section “Methods”), we derive the system of BS equations for the relevant vertex parts Γi (see Fig. 2). The starting Hamiltonian is:

Figure 2
figure 2

Diagrams for the system of Bethe-Salpeter equations.

Solid and dashed lines stand for hole and electron propagators, respectively. The SDW polarization loop contains one electron and one hole bare Green function. The Cooper loops Πs contain two electron or two hole bare propagators, respectively.

where fσk, cσk stand for annihilation operator in electron and hole bands; and μ are dispersions and chemical potential, respectively.

Based on the results of RG calculations33,34, we choose four vertices relevant to the s± coupling (the vertices u1, u3, u4 = us, u5 = us). The vertex u2 which has been shown to be irrelevant34 is excluded.

The vertices Γ1i with i = 1, 2 (see Fig. 2) describe the interactions in the density-wave block, the vertices Γ4,5 describe the singlet Cooper pairing in the electron and hole pockets, respectively, and the vertex part Γ3 includes the interactions responsible for the interband (e-h) Cooper pairing. The system of Bethe--Salpeter equations may be written in the symmetric form using a matrix :

The matrix is the secular matrix and

The secular equation for this system of Bethe-Salpeter equations for the modes

is . In these notations both coupling constants ui = νUi and the polarization loops Πi(q = 0, ω = 0) = ln(W/T) are dimensionless (here W is the bandwidth). We neglect below the difference between the band dispersion in the electron and hole pockets, when calculating the polarization operators Πs = Πse = Πsh. One should note that his approximation does not imply that we rely on perfect nesting. In electron doped materials the strict nesting conditions are of course violated, but the small difference between the electron and hole polarization operators is insufficient for our theory because two contributions are summed in the critical mode D32 which is central to our scenario. The criticality in this mode is dominated by the term u1Π1. We use the sign convention that both Π1 and Πs are positive. Under this convention us > 0 is attractive in the Cooper channel and u1 > 0 facilitates the instability in the SDW channel.

In the explicit form the secular equation reads:

One can see that in this approximation the triplet Γ31-channel described by the second row of the secular equation decouples from the rest, which corresponds to the - SDW and superconducting channels. The D32-mode plays a very particular role. On the one hand it contributes to the density wave channels (both CDW and SDW). On the other hand it strongly affects the superconducting channel. In the approximation used in the present paper the SDW and CDW are degenerate. The interband interaction u2 > 0 with momentum transfer Q lifts out the degeneracy favouring the SDW transition.

We will consider the part of the phase diagram concentration-temperature (c − T) close to the point of the degeneracy of the s± and SDW channels (i.e. the tetracritical point) shown in Fig. 1. In this region the SC instability takes place in the presence of critical SDW fluctuations. Above Ts the fluctuation modes arise at momenta p = Q + q close to the nesting vector Q connecting the Γ and X points in the Brillouin zone and at small ω → 0.

We assume that the two Cooper propagators D4 and D5 are far from any divergence, namely at these temperatures (in case of a dominant interband pairing mechanism as in the pronounced s± case adopted here, the purely intraband Cooper instabilities develop at temperatures much less than the actual Tc). In this approximation the vertices are real, and the channels 4, 5 are represented by a single row and column.

Away from the tetracritical point

We consider first the case when the temperature is less than the Fermi-energy T < εF and the doping c is away from the tetracritical point. Then the divergence of the vertices is strongly peaked at particular momenta. For instance, putting u3 → 0 in the integral equation for the Γ11(p1, p2, p3, p4) (see Fig. 2a), one immediately gets that this vertex is divergent only for p1 + p2 = Q. A similar analysis shows that Γ32 diverges for p1 + p2 → 0 and p1 − p3 → Q. The splitting of momenta, at which the vertices diverge, decouples the matrix Eq. (5) into the density-wave and Cooper channels. To study the properties of the vertex functions in the vicinity of their singularities we introduce , where and have poles at k, p → 0 correspondingly. For the vertices Γ32 and Γ4 we use the same decomposition: and .

To identify the corresponding transition temperatures we consider the Bethe-Salpeter equations in the static limit. For small momenta the system Eq. (5) splits up in the logarithmic approximation (see Section “Methods”) into cooper channel:

and density-wave channel

With these vertices we now calculate the susceptibility in the cooper and density-wave channels. In the particle-particle s± and s++ channel drawn in Fig. 3 we obtain

Figure 3
figure 3

Cooper and density waves susceptibilities.

The shaded boxes denote the corresponding combination of the vertices (see the text for details).

Substituting Eq. (9) into Eq. (11), we get:

This equation has the typical pole structure for the superconducting susceptibility in the vicinity to the transition temperature. The susceptibility increases with decreasing temperature and diverges at the critical transition temperature. This happens under condition 1 − (us ± u3s(k = 0, T = Tc) = 0. The two solutions correspond to s++ and s± superconducting order parameter. For CDW and SDW channels we get:

The SDW transition is determined by 1 − (u1 + u31(q = 0, Tc) = 0. One can define a tetracritical point, when both susceptibilities diverge. It happens under the condition (us + u3s(k = 0, Tc) = (u1 + u31(k, Tc) → 1. In this case and in the vicinity of the tetracritical point one should find the divergence of the susceptibility taking into account the full matrix Eq. (5).

Close to the tetracritical point: dynamical multi-mode coupling theory

Now we consider the interplay between magnetic and superconducting degrees of freedom in the vicinity of the tetracritical point. In this case the approach based on the effective hydrodynamic action is much easier than the direct solution of the BS equations. Besides, this approach which also accounts for the multi-point correlation functions goes beyond the conventional BS paradigm limited by two- and four-point Green’s function16,17. The derivation of the effective hydrodynamic action in terms of magnetic and superconducting (i = e, h) dynamical fluctuations is done by integrating out the BS equations with respect to the “fast” (with the energy of the order of the bandwidth) degrees of freedom and is presented in Section “Methods”.

Within our analysis we start discussing the limiting case and corresponding to the interplay between two fluctuating modes: one is the s± superconducting and another one is the SDW magnetic. This regime is believed to be present in most of FeSC [e.g., in broadly studies doped “A-122” systems (where A = Ba, Sr, Ca)] The Lagrangian of the two-mode coupling theory takes the form:

Here the Fourier transforms of superconducting and SDW fluctuators computed on Matsubara frequencies iΩm read:

Here ψ(x) and ψ′′(x) are the di-gamma function and its second derivative respectively, 〈...〉FS denotes the averaging over the Fermi surface (here a parabolic dispersion and equal mass were assumed for electron and hole pockets). The analytic continuation of the superconducting and SDW fluctuators to the upper half-plane iΩm → Ω + i0+ for is given by

Notice that we normalize the fluctuators by the density of states to make them dimensionless. The equations defining the coefficients A, B, C1, C2 and cΔ/m are derived in Section “Ginzburg-Landau approach”. The static q - independent part of the Lagrangian corresponds to the Landau expansion of the free energy. Inclusion of the gradient terms generalizes the Landau theory to the Ginzburg-Landau functional (see Section “Ginzburg-Landau approach”). The effective Lagrangian describes effective non-linear theory of interacting mode and therefore goes beyond linear Bethe - Salpeter approach. Hidden non-linearity of Bethe-Salpeter equations is associated with curved (“non-flat”) phase space: Γ32 enters both SDW and superconducting equations being singular both at small total moment/energy and small deviating from Q momentum transfer. The Lagrangian (14) is U(1) × SU(2) symmetric.

Although the situation in 1111 and 122 pnictides is described in the framework above, we consider for the sake of generality also the opposite limit u3us and usΠs ~ 1. In this case one deals with the three-mode coupling theory: two superconducting fluctuating modes Δe and Δh and one SDW magnetic mode:


As in the static case, we neglect the difference between the contribution of electron and hole pockets in the fluctuation modes. In principle, the SDW and CDW modes are degenerate when and one needs to consider a four-mode coupling theory. We however, assume that the SDW-CDW degeneracy is lifted out by additional inter-band processes u2 (see Eq. (4) and further details in refs 33, 34), omitted through the derivation of the BS equations, TCDW < Ts and restrict ourselves by the three-mode coupling theory.

The Lagrangian (17) at C2 = 0 (Fig. 4a–e) describes U(1) × U(1) × SU(2) gauge theory where each U(1) corresponds to the gauge symmetry of the superconducting (e- and h-) sectors and SU(2) represents the magnetic (SDW) sector of the effective model. The most important observation is that magnetic fluctuations (Fig. 4f,g) break U(1) × U(1) → U(1) and mediate the cross-talk between two different superconducting (e-h) sectors.

Figure 4
figure 4

Interaction between fluctuations: wavy lines represent the superconducting fluctuators Le/h(q, Ω, T), broken lines stand for magnetic (SDW) fluctuator Dm(q, Ω, T).

Diagrams (a,b) define A coefficient, (c) - B- coefficient, (d,e) - C1 - coefficient, (f,g) - C2 - coefficient. Notations for solid and dashed lines are the same as in Fig. 2.

Fluctuation corrections to Tc and Ts

In order to find the fluctuation correction to the superconducting transition temperature given by the mean-field analysis in the vicinity of the tetracritical point, we integrate out the remaining slow magnetic fluctuations in (14) and finally obtain the effective Lagrangian describing the superconducting system:


is the superconducting fluctuator renormalized by magnetic fluctuations. As a result, we find a fluctuation correction to Tc:

where is the transition temperature defined by the static solution of BS equations (mean-field theory) and

Here are bare Green’s Functions for electron/hole bands respectively. We observe that there are two types of competing processes: the one with +C1 leads to K1 > 0 and results in suppression of Tc while the second one with −C2 corresponds to K2 < 0 and therefore enhances Tc.

Similarly, for the second case described by the Lagrangian (17) characterized by magnetic fluctuation broken U(1) × U(1) we get the following effective Lagrangian

where the diagonal Δe − Δe and Δh − Δh inverse fluctuators and are given by the diagrams Fig. 5(a,b) while the off-diagonal Δe − Δh coupling K2 is defined by the diagrams Fig. 5(c,d). The corresponding equations for the d- dimensional cases (d = 2, 3) are given by:

Figure 5
figure 5

SDW fluctuation corrections to: e- and h- superconducting fluctuators (a,b), cross-coupled e-h terms (c,d). SC fluctuation corrections to the SDW fluctuators (e,f).

While the diagrams Fig. 5(a,b) always reduce the effective temperature of the superconducting transition, the diagrams Fig. 5(c,d) lift the degeneracy between e-h transition temperatures. As a result, assuming that K1e = K1h = K1, K2eh = K2 we get the fluctuation correction to the critical temperature Tc:

To construct the effective field theory for the influence of superconducting fluctuations on the SDW dynamics, we integrate out the slow superconducting fluctuations in (17) and finally obtain the effective Lagrangian for paramagnetic SDW fluctuations:

where for two-mode coupling theory with


while for three-mode coupling theory with

The diagrams defining the fluctuation corrections to Ts are shown on Fig. 5(e,f).

Computing the correcting terms for the three-mode coupling theory we obtain that the fluctuation correction to the SDW transition temperature always leads to its reduction:

Exactly at the tetracritical point , the concentration c = c0, . Due to the assumed particle-hole symmetry we get . Finally, combining (28) and (35) we get

and therefore the new tetracritical point corresponds to lower values of the concentration c < c0 (see Fig. 1).

Let us illustrate, as an example, the calculation of the fluctuation corrections diagrams K1,2 containing the superconducting fluctuator Le/h(q, Ω) (the evaluation of the diagrams containing the SDW fluctuator can be performed in a similar fashion). The evaluation of the Matsubara sums and integrals can be done in several steps:

(i) First, the main contribution to the sum over Ωm is given by the m = 0 term. Therefore we can replace

(ii) Second, we notice that the integral over q is determined by the small q: where ξs is the superconducting coherence length, for d-spatial dimensions d = 2, 3. We can therefore neglect the q-dependence in the e/h Green’s functions:

(iii) Next, the sum over fermionic Matsubara frequency εn and summation over k in K1 and K2 is performed in the same way as explained below in the Section “Ginzburg-Landau approach” (see Section “Methods”). As a result we obtain:

Notice, that after these approximations there is no difference between K1 and K2.

(iv) The remaining integral over momentum q is performed using the static Ornstein-Zernike correlator Le/h(q, 0) (see ref. 36)

here Vd denotes the unit volume. We see that for d = 3 the integral (39) is convergent,

Here we introduced the Ginzburg number Gi(d) defined as the range of reduced temperatures δT/Tc where the fluctuation corrections to the specific heat are comparable to its jump at Tc. For d = 3 the Ginzburg number . For d = 2 the integral (39) diverges logarithmically:

(v) Finally we replace τc in (41) by its low bound - the Ginzburg number (recall, that by its definition ) and substitute Gi(2) ~ T0/εF (see ref. 36 where similar calculations have been performed for a single U(1)-mode theory by means of Renormalization Group technique).

Performing similar calculations for the renormalization of the SDW critical temperature Ts we obtain:

We emphasize that the constants K1 and K2 characterizing the fluctuational shift of the critical temperature are found to depend on the Ginzburg number Gi(d) and the dimensionality of the system d only.

Eq. (42) represent the central result of the paper: fluctuation corrections are responsible for the competition between the spin density wave and superconducting critical modes in the vicinity of the tetracritical point. We have obtained this results by calculating the fluctuation corrections to the GL functional, but the same result may be obtained in the framework of renormalization group approach. Since the U(1) × U(1) symmetry is a priori broken in the superconducting sector of the model, the influence of the magnetic fluctuations onto the superconducting transition is two-fold: first, the intra-band corrections tempt to reduce the transition temperature; second - the inter-band corrections do exactly the opposite - split the two transition temperatures and effectively facilitate the superconducting transition. On the other hand, the contribution of superconducting fluctuations in the SU(2) magnetic sector of the model does result only in a suppression of the SDW transition. The contribution of “eigen” fluctuations, namely the superconducting-superconducting and magnetic-magnetic is alike and therefore it is dropped off from the difference of the critical temperatures. The asymmetric character of the fluctuation corrections results in the shift of tetracritical point towards lower values of the carriers concentration. For the “dirty” limit of the multi-mode coupling theory the Ginzburg numbers should be updated accordingly36.

The strong renormalizations of Tc and Ts are expected in iron based superconductors, which are rather two-dimensional and many of them have rather small Fermi energy. In these materials the value of the Ginzburg number may be quite large. For instance, the characteristic value of the Fermi energy in 1111 and 11 compounds is 100 meV38,39,40, while the superconducting critical temperature is about 20–50 K. With this numbers the one finds large Ginzburg number Gi(2) ~ Tc/εF ~ 0.02–0.05 and considerable renormalizations of the critical temperatures (Tc − Ts)/Tc ~ 0.1.


We have developed a high-temperature approach to the problem of interplay between magnetic and superconducting ordering in multi-band systems. Both static and dynamical (fluctuation related) contribution to the mode-mode coupling are discussed. It is shown that the fluctuation corrections in the vicinity of the tetracritical point reduce the magnetic transition in accordance with Eqs (32), (36). On the superconductor side of the phase diagram the situation is different. The intraband and interband contributions of spin fluctuations to the Ginzburg-Landau functional nearly compensate each other.

The approach that we have introduced is more general than for instance a mean-field description of competing phases4,5 as it accounts for dynamical fluctuations and goes beyond the static scaling paradigm. Apart from this, the framework presented here has the advantage that it can be generalized to other multi-mode regimes in a straightforward manner, which can include e.g. the presence of a nematic instability, the competition between s± and s++ and/or singlet/triplet pairings. Besides, it is highly appealing to discuss in a framework of this approach the influence of conventional magnetic defects (transition metal ions substituting for Fe) and weak magnetic defects produced by Zn impurities and As-vacancies on the superconducting transition temperature. This work is now in progress.


Integral Bethe-Salpeter equations

The integral Bethe-Salpeter equations in d = 2, 3 dimensions take the form

where we used the short-hand notations

, , with fermionic Matsubara frequencies ωn = εn = 2πT(n + 1/2) and bosonic Matsubara frequency Ωm = 2πmT and the irreducible vertices j0 include all irreducible diagrams in the channel j. The spin, momentum and energy are conserved in each vertex: p4 = p1 + p2 − p3. The simplified matrix BS equations are obtained by a replacement

Due to momentum conservation there are only three independent momenta. It worth to introduce new variables p = p1 + p2 = p3 + p4, q = p3 − p2 and t = p3 − p1. In the new variables the first integral in Eq. (43) has the form:

Considering the first equation one sees that the dependence on the first p and the last t variables is weak due to internal integrations over and can be substituted with log accuracy by the characteristic transfer momenta . It leads . Similar one finds . However, vertex depends on two variables due to couplings to the Cooper and the SDW channels. With this substitution and using the bare Green’s functions instead of dressed GF in the polarization loops, we obtain:

the Eq. (44) get a simplified form:

In the case of , SDW and SC channels are strongly coupled and have the same pole structure. With logarithmic accuracy for the two channels separate from each other.

Now let us consider the case of finite temperature away from tetracritical point . The system of equations with log accuracy reduces to the system:

which can be easily solved

Here the sign “+” corresponds to SDW channel, while the the sign “−” to CDW channel. The SDW magnetic instability develops when 1 − (u1 + u31(q) = 0. Close to the instability point it is naturally to expand near the SDW vector Q. Then 1 − (u1 + u31(Q + q, iΩn → Ω + i0+) τ + cmq2 − iΩ/γsdw (see also Section “Ginzburg-Landau approach”). It leads

Similar to above we consider the superconducting channel away from the tetracritical point:

where + corresponds to s± superconductivity, while − to s++. Close to the transition point for small q:

Effective action for the multi-mode theory: beyond the Bethe-Salpeter approach

We start with the Hamiltonian (4). Since superconducting and magnetic sectors are block-diagonal, let’s begin with description of the Gaussian action for two-band superconductor away from the magnetic phase:

As a first step we introduce fluctuating fields for description of the e- (f) and h- (c) superconductivity

The second step is to use an integral representation for the functional δ- functions

and the Lagrangian takes form


is a Nambu 2-spinor and

and and .

As a next step we compute Gaussian integral over Grassmann fields f and c. As a result,

Expanding in terms of fermionic loops one gets:

where expansion contains even number of the Green’s functions and for minimal mode-mode coupling theory it is enough to retain quadratic and quartic terms. Finally, computing the path integral over η's by the saddle point:

we arrive at the effective action describing fluctuating Cooper pairs:

The eigen modes of superconducting fluctuators are given by:

Two important limiting cases: (i) and - superconducting fluctuating modes are almost degenerate and basis represents correct basis for the multi-mode coupling theory; (ii) u3Πs ~ 1 and - superconducting fluctuation modes are spit onto s± and s++ modes, Tc for s± is higher and the new basis describes rotated by θ = π/4 old basis .

The magnetic part of action describing SDW fluctuations is obtained by similar way:

(i) we introduce the 2-spinor

(ii) we insert vector bosonic fields describing magnetic fluctuations by means of δ-function

(iii) implement the integral representation for the functional δ-function

The next steps are similar to derivation of superconducting fluctuating part: integrating over Grassmann variables and integrating over by means of the saddle point approximation. As a result, the magnetic fluctuators are described by the Lagrangian:

with fluctuator

Notice, that we excluded the CDW instability characterized by the fluctuator of CDW mode : due to lower TCDW < Ts.

Finally, we elaborate on the coupling between superconducting and magnetic modes. For this sake we need a “super-Nambu” 4-spinor

Performing a loop expansion (see Fig. 4) we get

where C1 and C2 are defined in the next section.

Ginzburg-Landau approach

In order to establish a correspondence between the microscopic fluctuation theory of competing modes and the macroscopic thermodynamic description, we can derive an effective Ginzburg-Landau (GL) functional. The GL functional for should be written in terms of order parameters corresponding to competing modes (see, e.g. refs 41, 42, 43, 44, 45).

We present the GL functional for two important cases discussed in the paper.

(i) the magnetic fluctuating mode is coupled to superconducting mode:

(ii) the magnetic fluctuating mode is coupled to two superconducting fluctuationg modes and :

The coefficients αΔ = ln(T/Tc) and αm = ln(T/Ts) change sign at the corresponding transition temperatures (in the case of the transition between the ordered states SDW or SC and the coexistent states, the closed loops are constructed from corresponding anomalous Green functions). The coefficients and in front of the gradient terms are obtained in a standard way from the small momentum expansion of the polarization loops Πs and Π1, ξs and ξm are superconducting and magnetic coherence lengths respectively (in the “dirty” limit the coherence length ξs/m should be replaced by where l is the mean-free path. This replacement changes the Ginzburg number accordingly), see details in ref. 16, 17, 36.

The fourth order terms are given by the loops containing four Green’s functions (see Fig. 4 and ref. 41).

and, as a result41

Note that the coefficient in front of the mixed term is different in the s++ (C++ = C1 + C2 = 3A) and s± (C+− = C1 − C2 = A) modes41.

Additional Information

How to cite this article: Kiselev, M. N. et al. Coupled multiple-mode theory for s± pairing mechanism in iron based superconductors. Sci. Rep. 6, 37508; doi: 10.1038/srep37508 (2016).

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