We consider finite-range effects when the scattering length goes to zero near a magnetically controlled Feshbach resonance. The traditional effective-range expansion is badly behaved at this point, and we therefore introduce an effective potential that reproduces the full T-matrix. To lowest order the effective potential goes as momentum squared times a factor that is well defined as the scattering length goes to zero. The potential turns out to be proportional to the background scattering length squared times the background effective range for the resonance. We proceed to estimate the applicability and relative importance of this potential for Bose-Einstein condensates and for two-component Fermi gases where the attractive nature of the effective potential can lead to collapse above a critical particle number or induce instability toward pairing and superfluidity. For broad Feshbach resonances the higher order effect is completely negligible. However, for narrow resonances in tightly confined samples signatures might be experimentally accessible. This could be relevant for suboptical wavelength microstructured traps at the interface of cold atoms and solid-state surfaces.

1. Introduction

Cold atomic gases have enjoyed many great successes since the first realizations of Bose-Einstein condensates in the mid nineties [1]. Ensembles of ultracold atomic gases can be manipulated in magnetic or optical trap geometries and in lattice setups, effectively mimicking the structure of real materials and teaching us about their properties. In particular, extreme control can be exercised over the atom-atom interactions through the use of Feshbach resonance [2]. Tuning the system into the regime of resonant two-body interactions provides a controlled way of studying strongly correlated dynamics which is believed to be crucial for material properties such as high-temperature superconductivity or giant magnetoresistance.

Recently there has been extended interest in weakly interacting Bose-Einstein condensates for use as an atomic interferometer [3] and also to probe magnetic dipolar interactions in condensates [4]. This work was based on 39K atoms where a broad Feshbach resonance exists at a magnetic field strength of 𝐵0=402.4G [5] which allows a large tunability of the atomic interaction in experiments [6]. Similar tunability has also been reported in a condensate of 7Li [7]. The atomic interaction can be reduced by tuning the scattering length, 𝑎, to zero, also known as zero crossing. In a Gross-Pitaevskii mean-field picture we can thus neglect the usual nonlinear term proportional to 𝑎. The question is then what other interactions are relevant. As shown in [4], the magnetic dipole will contribute here.

In the Gross-Pitaevskii picture we might also ask whether higher order terms in the interaction can contribute around zero crossing. Recently it was shown that effective-range corrections can in fact influence the stability of condensates around zero crossing [8–10]. The Feshbach resonances used thus far in experiments have typically been very broad, and as a result the effective range, 𝑟𝑒, will be small, rendering the higher order terms negligible. However, around narrow resonances this is not necessarily the case and finite-range corrections are not necessarily negligible.

For the two-component Fermi gas, there has been increased interest in producing a cold atom analog of the celebrated Stoner model of ferromagnetism [11] which applies to repulsively interacting fermions. Theoretical proposals indicate that this should be possible [12–19], and an MIT experiment subsequently announced indications of the ferromagnetic transition [20]. The results caused controversy since the spin domains were not resolved [21–24]. A later experiment in the same group did not find evidence of the ferromagnetic transition [25]. However, these studies consider broad Feshbach resonances, and the situation with narrow resonances is less clear. One can imagine that finite-range corrections could play a role in driving the phase transition. In fact, a recent experiment in Innsbruck [26] has found increased lifetimes of the repulsive gas in the strongly imbalanced case, providing hope that decay into molecules can be controlled and ferromagnetism can be studied.

The systematic inclusion of finite-range effects through derivative terms in zero-range models was begun in the study of nuclear matter decades ago [27, 28]. Later on the intricacies of the cut-off problems that arise in this respect were considered by many authors both for the relativistic and nonrelativistic case (see [29] for discussion and references). In the context of cold atoms and Feshbach resonances, we need to use a two-channel model [30] in order to take the lowest order finite-range term into account. Similar models were already introduced in [31] and denoted resonance models (see f.x. [32] for a comprehensive review of scattering models for ultracold atoms). We note that whereas resonance models treat the closed-channel molecular state as a point boson the model of [30] treats the molecule more naturally as a composite object of two atoms. In the end the parameters of the two models turn out to be similarly related to the physical parameters of Feshbach resonances (see for instance the discussion of resonance models in [32]).

In Figure 1 we show calculations of scattering length and effective range for the Feshbach resonance at 𝐵=202.1 G in 40K in both a coupled-channel model [33] and in the zero-range model discussed here. We see the effective range being roughly constant at resonance and then start to diverge at zero crossing. The zero-range model provides a good approximation to the full calculations and for many-body purposes it is preferable due to its simplicity.

Whereas the earlier work of [31] considered the regime close to the resonance, we will be exclusively concerned with zero crossing. To our knowledge the intricacies of this region have not been addressed in the literature in the context of Feshbach resonances. Around zero crossing the Feshbach model turns out to have a badly behaved effective-range expansion. The parameters obtained from the effective-range expansion should therefore be used with extreme caution as the series is divergent at this point. However, as we show in this paper, the finite-range corrections obtained from the full 𝑇-matrix at low momenta via an effective potential turn out to be the same as one would naively expect based on the effective-range expansion. After introducing the effective potential we consider its applicability and importance in the case of Bose-Einstein condensates and for two-component Fermi gases where the attractive nature of the effective interaction at zero crossing could lead to collapse above a certain critical particle number or to pairing instability and superfluidity. In general, we find that tight external confinement is a necessary condition for the higher order effects to dominate the magnetic dipole interaction and be experimentally observable.

2. Two-Channel Model

We consider a two-channel 𝑠-wave Feshbach model with zero-range interactions [30] for which the on-shell open-open channel 𝑇-matrix as a function of magnetic field, 𝐵, is 𝑇𝑜𝑜(𝐵)=4𝜋ℏ2𝑎/𝑚𝑏𝑔ℏ1+Δ𝜇Δ𝐵/2𝑞2/𝑚−Δ𝜇𝐵−𝐵0−1+𝑖𝑎𝑏𝑔𝑞,(1) where Δ𝜇 is the difference between the magnetic moments in the open and closed channel, 𝑞 is the relative momentum of the atoms of mass 𝑚, 𝑎𝑏𝑔 is the scattering length away from the resonance at magnetic field 𝐵0, and Δ𝐵 is the width of the resonance. We can compare this to the standard vacuum expression for the 𝑇-matrix in terms of the phase-shift given by 𝑇𝜈=4𝜋ℏ2𝑎/𝑚−𝑞𝑎cot.𝛿(𝑞)+𝑖𝑎𝑞(2)

Typically, one has the low-energy expression −𝑞cot𝛿(𝑞)→−1/𝑎 which implies that 𝑇𝜈⟶4𝜋ℏ2𝑎/𝑚1+𝑖𝑎𝑞⟶0.(3) However, as we now discuss, for the realistic two-channel 𝑇-matrix for Feshbach resonances, the quantity −𝑞cot𝛿(𝑞) is not well defined, and the conclusion that the 𝑇-matrix vanishes at zero crossing is only true for zero momentum, 𝑞=0, as we now discuss.

From (1) and (2) we obtain the relation for the phase-shift: 𝑞cot𝛿(𝑞)=−1𝑎𝑏𝑔1+Δ𝜇Δ𝐵ℏ2𝑞2/𝑚−Δ𝜇𝐵−𝐵0−1.(4) We now expand the right-hand side in powers of 𝑞 as is usually done in an effective-range expansion. This yields 𝑞cot𝛿(𝑞)=−1𝑎+(𝐵)∞𝑛=1−1𝑎𝑏𝑔−𝑎𝑏𝑔𝑟𝑒02𝑛𝑎𝑏𝑔𝑎(𝐵)−1𝑛+1𝑞2𝑛,(5) where 𝑎(𝐵)=𝑎𝑏𝑔(1−Δ𝐵/(𝐵−𝐵0)) is the common parametrization from single-channel models and 𝑟𝑒0=−2ℏ2/(𝑚Δ𝐵Δ𝜇𝑎𝑏𝑔) is the background value of the effective range around the resonance. From (5) we can now read off all coefficients in an effective-range expansion with their full 𝐵-field dependence. For instance, the effective range is given simply by 𝑟𝑒=𝑟𝑒0[(𝑎𝑏𝑔/𝑎)−1]2, which is divergent when 𝑎(𝐵)→0. We also clearly see that all the other coefficients are divergent in that limit. This is signaled also before doing the full expansion in 𝑞 as the first term in (5) diverges at zero crossing. However, in effective potentials derived from the 𝑇-matrix these problems are not transparent as the lowest order coefficient is proportional to 𝑎(𝐵) (see (12)). Below we will discuss what kind of constraints this introduces on the applicability of the effective-range expansion near zero crossing. We note that similar issues were briefly discussed in a different context in [34] where an equivalent to (7) below was obtained.

Let us first consider the low-𝑞 limit and compare the full 𝑇-matrix with the effective-range expansion as zero crossing is approached. Taking the low-𝑞 limit of (4) at zero crossing where Δ𝐵/(𝐵−𝐵0)=1, we find 𝑞cot𝛿(𝑞)⟶−1𝑎𝑏𝑔−Δ𝜇Δ𝐵ℏ2𝑞2,/𝑚(6) which diverges as 𝑞−2. Therefore the coefficients of the expansion in (5) must necessarily diverge in order to retain any hope of describing the low-𝑞 behavior. Furthermore, since the expansion is an alternating series and therefore slowly converged, we also conclude that many terms must be retained for a fair approximation at very small but nonzero 𝑞. The same conclusion can be reached by considering the radius of convergence of (5), which we find by locating the pole in (4) at ℏ2𝑞2/𝑚=Δ𝜇(𝐵−𝐵0−Δ𝐵). This radius indeed goes to zero at zero crossing. We are thus forced to conclude that the effective-range expansion breaks down near zero crossing.

2.1. Effective Potential at Zero Crossing

Since the effective-range expansion is insufficient we consider the full 𝑇-matrix in the low-𝑞 limit at zero crossing. To lowest order we have 𝑇𝑜𝑜𝐵=𝐵0+Δ𝐵=−4𝜋ℏ2𝑎𝑏𝑔𝑚ℏ2𝑞2𝑞𝑚Δ𝜇Δ𝐵+𝑂4.(7) Using the expression for 𝑟𝑒0, this can be written 4𝜋ℏ2𝑚𝑎2𝑏𝑔𝑟𝑒02𝑞2.(8) Knowing the 𝑇-matrix at low 𝑞 we can now proceed to find an effective low-𝑞 potential through the Lippmann-Schwinger equation: 𝑉=𝑇−𝑇𝐺0𝑉,(9) where 𝐺0=(𝐞−𝐻0+𝑖𝛿)−1 is the free space Green’s function [35]. This equation can be solved for 𝑇(𝑞,𝑞′)∝𝑞2+𝑞′2 (the symmetrized version of the full 𝑇-matrix) in an explicit cut-off approach [29, 35] and then be expanded to order 𝑞2 for consistence with the input 𝑇-matrix. In the long-wavelength limit we can take the cut-off to zero [35] and for the on-shell effective potential we then obtain the obvious answer: 𝑉(𝑞)=4𝜋ℏ2𝑚𝑎2𝑏𝑔𝑟𝑒02𝑞2(10) in momentum space. The effective potential in real-space is now easily found by canonical substitution (𝐪→−𝑖∇) and appropriate symmetrization [36]. We have 𝑉(𝐫)=−4𝜋ℏ2𝑚𝑎2𝑏𝑔𝑟𝑒0212←∇2𝐫𝛿(𝐫)+𝛿(𝐫)→∇2𝐫.(11) Notice that the Lippmann-Schwinger approach is nonperturbative as opposed to the perturbative energy shift method [36, 37].

2.2. Comparison to Effective-Range Expansion and Energy-Shift Method

Away from zero crossing one can easily relate the effective-range expansion to an effective potential through the perturbative energy shift method [18, 25, 26]. To second order the 𝑠-wave effective potential is 𝑉(𝐫)=4𝜋ℏ2𝑎𝑚𝑔𝛿(𝐫)+22←∇2𝐫𝛿(𝐫)+𝛿(𝐫)→∇2𝐫,(12) where the first term is the effective interaction usually employed in mean-field theories of cold atoms [35]. In terms of 𝑎 and 𝑟𝑒, we have 𝑔2=𝑎2/3−𝑎𝑟𝑒/2 [36, 37] with the field-dependent 𝑎=𝑎(𝐵) and 𝑟𝑒=𝑟𝑒(𝐵).

At zero-crossing the first term in (12) vanishes and one might expect the second term to vanish as well. However, in the naive effective-range expansion of the two-channel model discussed above we saw that 𝑟𝑒 diverges as 𝑎−2 and we therefore have lim𝑎→0𝑎𝑔2𝑎=−2𝑏𝑔𝑟𝑒02.(13) In particular, if we for a moment ignore 𝑞4 terms in the effective-range expansion, we recover exactly the same effective potential as in (11) at zero crossing. The finite limiting result in (13) shows that the potential in (12) is well defined as 𝑎→0, provided that appropriate regularization and renormalization are performed. Equation (12) thus applies equally well at resonance (𝑎→∞) where the gradient terms are small and at zero crossing where the lowest order delta function term is unimportant. It is thus a well-defined effective potential over the entire range of a Feshbach resonance.

We therefore see that even though the effective-range expansion has divergent coefficients at zero crossing, the lowest order does in fact give the same effective potential as the full 𝑇-matrix if we apply it naively. The effective-range expansion should thus be viewed as an asymptotic series. However, we cannot use the effective-range expansion to estimate the validity of the second-order effective potential since the radius of convergence goes to zero at zero crossing as discussed above.

The two-channel model in (1) compares well with a coupled-channel calculation [33] as shown in Figure 1. It also compares well to other scattering models [38, 39] that include finite-range effects. In fact, the model used here compares well with the analytical models of [38] when 𝑎(𝐵) and 𝑟𝑒(𝐵) have the field-dependence introduced above. This can be seen for instance in Figure 12 of [38], although a difference is that our 𝑎(𝐵) and 𝑟𝑒(𝐵) are parametrization and not taken from coupled-channels values as in [38] (our Figure 1 quantifies the difference which is largest on 𝑟𝑒(𝐵)). However, here we are concerned with the behavior when 𝑎(𝐵)→0 in the context of Feshbach resonances which is not addressed in [38, 39]. We note that the resonance models of [31] and the two-channel and resonance models in [32] are very similar to the model employed here, but again those references do not consider the specific problems arising when 𝑎(𝐵)→0. In addition and in contrast to previous discussions, here we construct appropriate zero-range pseudo potentials that work around zero crossing.

3. Relation to Experiments

Above we only retained terms of order 𝑞2 in the full 𝑇-matrix. We now estimate the energy regime in which this expression is valid. Demanding that the 𝑞4 term be smaller than the 𝑞2 term gives the criterion: ℏ2𝑞2𝑚≪ℏ2𝑚||𝑎𝑏𝑔𝑟𝑒0||.(14) We relate this condition to recent experiments with bosonic condensates of 39K working around zero crossing [3]. The resonance used there is very broad (Δ𝐵=−52G) with 𝑎𝑏𝑔=−29𝑎0 and 𝑟𝑒0=−58𝑎0 (𝑎0 is the Bohr radius). The right-hand side of (14) is 2.3⋅10−7 eV, corresponding to a temperature of about 3 mK. Since the experiments are performed at much lower temperatures the approximation above is certainly valid. However, as 𝑎𝑏𝑔 and particularly 𝑟𝑒0 are small, the front factor in (11) is also small. The relevant scale of comparison is the outer trap parameter 𝑏 [9] which is typically of order 1 Όm, yielding a vanishing ratio |𝑎2𝑏𝑔𝑟𝑒0|/𝑏3∌10−9. For broad Feshbach resonances the higher order interactions can thus be safely ignored. For very narrow resonances the situation potentially changes as 𝑟𝑒0 can be very large and make the potential in (11) important. As an example, we consider the narrow resonance in 39K at 𝐵0=25.85G with Δ𝐵=0.47G, 𝑎𝑏𝑔=−33𝑎0, and 𝑟𝑒0=−5687𝑎0 [5]. The right-hand side of (14) is now 2⋅10−9 eV, corresponding to 24 ΌK. This is again much higher than experimental temperatures. A more careful argument can be made from the energy per particle of the noncondensed cloud. Ignoring the trap, we have 𝐞/𝑁=0.770𝑘𝐵𝑇𝑐(𝑇/𝑇𝑐)5/2 (𝑇𝑐 is the critical temperature) [35]. For a sample of 3⋅104 a critical temperature of 100 nK was reported in [6]. Using this 𝑇𝑐 we find that 𝑇≪900 nK for (14) to hold. Again this is within the experimental regime. The effective potential approach should therefore be applicable around zero crossing for narrow resonances. However, even with this narrow resonance we find |𝑎2𝑏𝑔𝑟𝑒0|/𝑏3∌10−7, and the effect is still completely negligible.

In order to increase the relevance of the higher order term, we now consider some very narrow resonances that have been found in 87Rb. In particular, the resonance at 𝐵0=9.13G [40] which was recently utilized in nonlinear atom interferometry [41]. We have Δ𝐵=0.015G, 𝑎𝑏𝑔=99.8𝑎0, and Δ𝜇=2.00𝜇𝐵 [42], which gives 𝑟𝑒0=−19.8⋅103𝑎0 and a ratio |𝑎2𝑏𝑔𝑟𝑒0|/𝑏3=2.92⋅10−5(1𝜇m/𝑏)3. A trap length of 𝑏∌0.5 Όm as used in [41] would thus yield 10−4 and demonstrates that higher order corrections can safely be neglected. For a ratio of 1 we need 𝑏∌0.03 Όm which is unrealistically small in current traps or optical lattices. However, a resonance of width Δ𝐵=0.0004G is known in the same system at 𝐵0=406.2G [43] with 𝑎𝑏𝑔=100𝑎0 and Δ𝜇=2.01𝜇𝐵 [42]. In this case we find 𝑟𝑒0=−7.4⋅105𝑎0 and a much more favorable ratio of |𝑎2𝑏𝑔𝑟𝑒0|/𝑏3=0.001(1𝜇m/𝑏)3. Here we see that a ratio of 1 is achieved already for 𝑏∌0.1𝜇m which not far off from tight traps or optical lattice dimensions. In terms of temperature we still have to be in the ultralow regime of 𝑇≲30nK according to (14) for the latter resonance.

Consider now a fermionic two-component system where 𝑠-wave interactions are dominant. Since we have 𝑟𝑒0<0 for all Feshbach resonances [42], the effective potential in (10) is attractive, and the system could potentially be unstable toward a paired state or become unstable to collapse above a critical particle number. For simplicity we will use the semiclassical Thomas-Fermi approach to describe a gas with equal population of the two components and estimate the critical particle number. Assuming an isotropic trapping potential with length scale √𝑏=ℏ/𝑚𝜔 where 𝜔 is the trap frequency, the ground-state density, 𝜌(𝐱), can be found by minimization and satisfies 𝜇−1ℏ𝜔2𝐱𝑏2=12𝑘𝐹(𝐱)𝑏2−4𝛌𝑘30𝜋𝐹(𝐱)𝑏5,(15) where 𝜌(𝐱)=𝑘𝐹(𝐱)/6𝜋2 and 𝛌=𝑎2𝑏𝑔|𝑟𝑒0|/𝑏3. The maximum allowed momentum and chemical potential, 𝜇, is found by solving for the turning point of the right-hand side of (15) which gives 𝑘max𝑏=3𝜋2𝛌1/3,𝜇max=3𝑘10ℏ𝜔max𝑏2.(16) We can now compare this 𝑘max to the value obtained from the noninteracting density within the Thomas-Fermi approximation at the center of the trap. In terms of the number of particles in each component, 𝑁, at the center of the trap we have 𝑘𝐹(0)𝑏≈1.906𝑁1/6 [35]. By equating these two expression we obtain an estimate for the critical number of particles, 𝑁max. Inserting the relevant units, we have 𝑁max=2⋅1025𝑎0𝑎𝑏𝑔4𝑎0𝑟𝑒02𝑏1𝜇m6,(17) where 𝑎0 is the Bohr radius. We note that the scaling 𝑁max∝𝛌−2 can also be obtained by considering the point at which the monopole mode becomes unstable.

Typical numbers for common fermionic species 6Li or 40K in the lowest hyperfine states [42] lead to 𝑁max∌1012 for 𝑏=1 Όm. This is of course a huge number and experiments are well within this limit. Even if one reduced the trap length by a factor of ten and made the presumably unrealistic assumption that the particle number remains the same we still have 𝑁≪𝑁max. The reason is that the 𝑠-wave Feshbach resonances utilized in the two-component gases are generally broad in order to study the universal regime. If we consider the narrow resonance at 𝐵0=543.25G in 6Li [44] with Δ𝐵=0.1G, 𝑎𝑏𝑔=60𝑎0, and Δ𝜇=2.00𝜇𝐵 [42], we have 𝑁max∌2⋅1013(𝑏/1𝜇m)6. This is somewhat better but we still need 𝑏∌0.06 Όm to get to an experimentally relevant 𝑁max∌106. We have to conclude that higher order 𝑠-wave interactions are highly unlikely to be observable through monopole instabilities. In light of this it seems better to consider 𝑝-wave resonances which are much more narrow in general. However, also here extremely small trap sizes appear necessary [45].

The instability toward Cooper pairing around zero crossing can also be estimated in simple terms. In general the critical temperature is 𝑇𝑐∌𝑇𝐹exp(−1/𝑁0|𝑈|), where 𝑁0=𝑚𝑘𝐹(0)/2𝜋2ℏ2 is the density of states at the Fermi energy in the trap center and 𝑈<0 is a measure of the attraction. For the latter we use the effective potential in momentum space from (10) and make the assumption that 𝑞∌𝑘𝐹(0). Using the expression for 𝑘𝐹(0) in terms of 𝑁 above, we find 1𝑁0||𝑈||=1.5⋅1012√𝑁𝑏1𝜇m3𝑎0𝑎𝑏𝑔2𝑎0||𝑟𝑒0||.(18) For broad resonances in 6Li or 40K this exponent is of order 103 and 𝑇𝑐 is thus vanishingly small. However, the scaling with trap size can help and if we imagine reducing to 𝑏=0.1 Όm, we find 𝑇𝑐≲0.5𝑇𝐹 for 𝑁=106 atoms. For the narrow resonance in 6Li discussed above, we find that 𝑇𝑐∌0.5𝑇𝐹 with 𝑁=106 can be achieved for 𝑏∌0.5 Όm and 𝑇𝑐∌0.1𝑇𝐹 for 𝑁=105. Thus there may be a possibility to reach the pairing instability near zero crossing if high particle numbers can be cooled in tight traps and narrow resonances are used.

While the suboptical wavelength trapping sizes needed for the above effects to be large are not achievable with typical optical or magnetic traps or optical lattice setups, they could potentially be reached via hybrid setups where atoms are trapped near a surface. Inspired by surface plasmon subwavelength optics [46], nanoscale trapping for neutral atoms has been studied [47, 48], and micropotential traps with width less than 100 nanometer (<0.1 Όm) are within reach [49]. In these very tightly confined systems, it is very likely that finite-range effects could be enhanced. Devices that provide an interface between atoms and solid-state systems are under intense study at the moment, and our considerations here imply that finite-range corrections should be considered when the scattering length is tuned close to zero.

3.1. Dipole-Dipole Interactions

The discussion above ignores the dipole-dipole interaction discussed in the introduction which will compete against the higher order effective potential from the Feshbach resonance. A simple estimate can be made along the lines of the discussion in [35]. The external trapping potential is the characteristic scale of spatial variations and we thus find a ratio, 𝑟, of magnetic dipole-dipole, 𝑈md, to higher-order 𝑠-wave zero-range interaction strength, 𝑈2, which can be written as 𝑈𝑟=md𝑈2=𝑎0𝑏2𝑎2𝑏𝑔||𝑟𝑒0||𝑏=35.71𝜇m2100𝑎0𝑎𝑏𝑔21000𝑎0||𝑟𝑒0||.(19) For 𝑟<1 the higher order interaction term will therefore dominate the magnetic dipole term. For the case of narrow resonances in 87Rb discussed above we find 𝑟∌0.11(𝑏/1𝜇m)2 for the resonance at 𝐵0=9.13G and 𝑟∌0.05(𝑏/1𝜇m)2 for the one at 𝐵0=406.2G. For the narrow resonance in 6Li at 𝐵0=543.25G we find 𝑟∌1.4(𝑏/1𝜇m)2. These ratios clearly indicate that magnetic dipole-dipole interactions can be suppressed relative to higher order zero-range terms for narrow Feshbach resonances and standard trap sizes. This dominance becomes even stronger for the tight traps needed for the realization of the effects discussed above, and we thus conclude that interference of the magnetic dipole-dipole term is not a major concern.

4. Conclusions and Outlook

In this paper we have discussed the effective potential around a Feshbach resonances as the scattering length is tuned to zero and finite-range corrections become important. We showed that the effective-range expansion is badly behaved and the effective potential most be defined from the 𝑇-matrix. We have demonstrated that the low momenta effective potential obtained from the full 𝑇-matrix agrees with one obtained naively from the effective-range expansion when the scattering length goes to zero. Thus even though the effective-range expansion has divergent coefficients at zero-crossing the first terms of the associated effective potential yield consistent results. We then estimated the effects of the terms on different condensates. Since the effective potential at zero crossing is attractive it may induce various instabilities which we considered for the case of a two-component Fermi gas under harmonic confinement.

For the broad Feshbach resonances used in current experiments the effective potential discussed here are negligible and the dipole-dipole interaction dominates completely at zero crossing. However, for narrow resonances in very tightly confined systems some of the effects might be detectable. In particular, future generations of microtraps with suboptical wavelength trap sizes using surface plasmons could be small enough to make finite-range effects important. The competing dipole interaction is small for narrow resonances in tight confinement. However, it is conceivable that effects of spherically symmetric higher order terms could be separated from dipolar effects which change with system geometry [4].

Small trapped Fermi systems have recently become an experimental reality with particle numbers ranging from two to ten [50]. For two atomic fermions with different internal states, the system turns out to be well described by the analytic zero-range model of Busch et al. [51–56], and similarly for three fermions [57, 58]. Effective-range corrections to these results have also been studied [59–62]. Mesoscopic Fermi systems (less than about 50 particles) have been studied in harmonic traps using a number of numerical methods, [63–79] with particular emphasis on the unitary regime where the scattering length diverges. It would be interesting to investigate the situation also around zero-crossing of a narrow resonance where the effective range is sizable. A preliminary study along this line for three bosons is discussed in [80].

Another interesting direction of future work is the study of the contact introduced by Tan [81–90] to describe the universal behavior of strongly interacting quantum gases at a broad resonance where the range corrections are negligible, for instance through the tail of the momentum distribution which is predicted to behave as 𝐶/𝑘4, where 𝐶 is the contact and 𝑘 the momentum of a single particle. The relations found by Tan [81, 82] have subsequently been confirmed experimentally in three dimensions [91–93]. While the contact originally pertains to two-body correlations, signatures of three-body physics in momentum distributions have also been studied both theoretically [86, 94–98] and experimentally [99]. While a few studies have considered the universal behavior when including the effective range term [100, 101], it would be very interesting to consider the regime around zero crossing for a narrow resonance where the background effective range parameter.


The author would like to thank Martin ThÞgersen for very fruitful collaborations. Correspondence with Georg Bruun about two-channel models is highly appreciated. The author is grateful to Nicolai Nygaard for discussions and for producing Figure 1. The author acknowledges the hospitality of the Niels Bohr Institute, Blegdamsvej 17, 2100 Copenhagen Ø, Denmark. This work was supported by the Villum Kann Rasmussen foundation.