Testing the Gaussianity and Statistical Isotropy of the Universe
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Review of Local NonGaussianity from Multifield Inflation
Abstract
We review models which generate a large nonGaussianity of the local form. We first briefly consider three models which generate the nonGaussianity either at or after the end of inflation; the curvaton scenario, modulated (p)reheating, and an inhomogeneous end of inflation. We then focus on ways of generating the nonGaussianity during inflation. We derive general conditions which a product or sum separable potential must satisfy in order to generate a large local bispectrum during slowroll inflation. As an application, we consider twofield hybrid inflation. We then derive a formalism not based on slow roll which can be applied to models in which the slowroll parameters become large before inflation ends. An exactly soluble twofield model is given in which this happens. Finally, we also consider further nonGaussian observables, a scale dependence of and the trispectrum.
1. Introduction
There are many models of the universe which can predict a large nonGaussianity. However the predicted amplitude and the shape of the nonGaussianity are different among different classes of models. One category is those which generate the nonGaussianity due to nontrivial classical dynamics on superhorizon scales. These models predict the shape of the bispectrum to be of the socalled “local type”, which can be expressed as an expansion of the Bardeen potential [1] where is the curvature perturbation on a Newtonian slice and is its linear and Gaussian part. denotes the ensemble average in a statistically homogeneous distribution. The current limit on the local type of the nonlinearity parameter from seven years of WMAP data [2] is at the 95% confidence level. Constraints are expected to improve rapidly and significantly, first with Planck data and later using large scale structure data, see the recent reviews [3–5]. The Bardeen potential is related to the primordial curvature perturbation of on large scales and in the matter dominated era by .
The curvature perturbation at horizon exit is determined by the classical perturbations of the scalar fields, . The subsequent evolution of can be conveniently described by the formalism [6–11]. The curvature perturbation is given by up to quadratic terms [11] where is the efolding number evaluated in an unperturbed Universe, from the epoch of horizon exit to later epoch of uniform energy density hypersurface (for an extension to include gradient terms, see [12]). The power spectrum and the bispectrum are defined by From this, we can define the observable quantities, the spectral index, the tensortoscalar ratio, and the nonlinearity parameter where is the power spectrum of the tensor metric fluctuations. It is well known that singlefield inflation does not lead to a detectably large nonGaussianity, in fact is suppressed by slowroll parameters [13]. Observably large nonGaussianity can be obtained by breaking the slowroll conditions during inflation [14], using extended kinetic terms [15–25], see also the reviews [26, 27], or going beyond models of singlefield inflation [11, 28–34]
It is natural to consider multiple scalar field since they are ubiquitous in many beyond the standard model of particle physics, such as supersymmetry and string theory. These scalar fields generate nonadiabatic perturbations during inflation and change the evolution of the curvature perturbation after horizon exit. The residual isocurvature perturbation may be present in the primordial density fluctuation and can be correlated with the curvature perturbation or may be responsible for an observably large nonGaussianity in the cosmic microwave background and large scale structure, for observational limits on isocurvature perturbations see [1, 35, 36]. In this paper, we will only consider models with adiabatic primordial perturbations, in which the isocurvature perturbation present during inflation is converted into an adiabatic perturbation. We also neglect the secondary nonGaussianities generated at later times, for example see [37, 38].
There are popular multifield models [39] which may generate observably large nonGaussianity. These include the curvaton scenario, modulated (p)reheating, and an inhomogeneous end of inflation, see Section 2. In these scenarios, large nonGaussianity is generated either by the means of ending inflation, or after inflation. It was shown recently that it also possible to generate large nonGaussianity during the evolution of slowroll multifield inflation, see Section 3.
All of these models generate the large nonGaussianity after horizon exit, such as after reheating, at the end of inflation, at the phase transition, or during inflation after horizon exit and involves the perturbation of the nonadiabatic mode. Therefore, the nonGaussianity of these models is of the local type which is distinguishable from other shapes of nonGaussianity (for a list of possibilities see, e.g., [40–42]), in which the nonGaussianity is generated intrinsically from the quantum fluctuations, or during horizon exit.
In Section 2, we summarise the aforementioned three models, which are popular methods of generating a large nonGaussianity. In Section 3, we review the possibility of generating a large nonGaussianity from multifield slowroll inflation, and in Section 4, we consider hybrid inflation with two inflaton fields as an application. Then in Section 5, we discuss multifield models of inflation without assuming the slowroll conditions and present an exact solution. NonGaussian observables beyond , such as its scale dependence and the trispectrum are introduced in Section 6. Finally, we conclude in Section 7.
2. Summary of Popular Models Generating a Large Local NonGaussianity
Multifield inflationary models [39] can lead to an observable signature of nonGaussianity. These include models in which the large nonGaussianity is generated either by the means of ending inflation, or after inflation. We review the three most popular of these models in this section, for a discussion on how these models are related see [43]. In the next section, we review the possibility of generating large nonGaussianity during multifield slowroll inflation. Later in Section 5, we discuss multifield models of inflation without assuming the slowroll conditions. This does not exhaust all of the possible ways of generating a large local nonGaussianity from inflation, see also the reviews [44–47] and the papers [48, 49]. NonGuassianity of the local form can also be generated in the ekpyrotic scenario [50, 51], although in the simplest case is large and negative [52], which is observationally ruled out.
2.1. Curvaton Scenario
In this scenario, there is a light weaklyinteracting inhomogeneous scalar field, the curvaton , in addition to the inflaton field, . The additional scalar field is completely subdominant during inflation however, it can dominate the energy density of the Universe later since the timeaveraged equation of state becomes that of the pressureless matter (), whose energy density decreases more slowly than that of the radiation which the inflaton field has decayed into. After decay, the inhomogeneity of the scalar field leads to the density perturbation of radiation [53, 54]. This is the basis of the curvaton scenario [55–59] which liberates the inflaton field from being required to generate the observed spectrum of perturbations (although there is instead an upper bound on their allowed magnitude).
The significant nonGaussianity of the local type can be generated in the curvaton model [60]. A study of nonGaussianity in the curvaton scenario using secondorder cosmological perturbation theory was done by Bartolo et al. [31] with a sudden decay approximation and also by Malik and lyth [32] using a fully numeric approach, which accounted for both the sudden decay and nonsudden decay approximations. Lyth and Rodríguez [11] used the formalism including the quadratic terms (second order terms in (2)) to calculate the nonGaussianity. The nonlinear generalisation of the curvature perturbation and a numerical study was done to give a full probability distribution function in [61]. This simple curvaton model was extended into the mixed curvatoninflaton scenario in which fluctuations of both the inflaton and a curvaton contribute to the primordial density perturbation studying the isocurvature perturbation in [62]. The multiple curvaton fields which contribute to the primordial density perturbation was studied in [63–65]. Observational constraints on curvaton models with isocurvature perturbation and nonGaussianity can be found in [66–68].
The generation of large nonGaussianity in the curvaton scenario can be easily understood using the result of the nonlinear formalism [61, 62]. Assuming the sudden decay of the curvaton field on the uniform energydensity hypersurface, that is, when the local Hubble rate equals the decay rate for the curvaton, leads to a nonlinear relation between the local curvaton density and the radiation density before and after the decay where . Here, is the primordial curvature perturbation which remains constant on large scales in the radiationdominated era after the curvaton decays and is the curvaton perturbation. Expanding this equation order by order yields up to second order [61] where at the time of the curvaton decay. The curvature perturbation of curvaton field [61] is almost constant before the curvaton decays from the start of curvaton oscillation. Note that the intrinsic nonGaussianity in the curvaton field during oscillation is , which comes from the nonlinear relation between and . After the curvaton decays into radiation, the curvature perturbation of radiation has the following nonGaussianity parameters: [11, 31, 61] where is evaluated when the curvaton decays based on the sudden decay approximation but gives good agreement with a full numerical study [32, 61], and is defined as In the limit of the pure curvaton scenario, , it recovers the usual normalization for , that is, . Therefore, the large is obtained for small . This large , in spite of the order of unity nonGaussianity in , has the origin in the nonlinear relation between (or ) and in (8).
In fact (7), and thus (8), can be used “at any time” before the curvaton decay with evaluated at that time to find the total curvature perturbation at that moment, as well as at the epoch of curvaton decay. This enables us to understand the evolution of the curvature perturbation on the uniform energy density hypersurface before the curvaton decay. Initially when the primordial radiation was generated, for example, from the inflaton decay, is negligibly small so we cannot ignore the perturbations of the inflaton field. At this early time, and since which makes negligible in (10). As time goes on, increases while and are almost constant since there is no energy flow between two fluids satisfying adiabatic condition except around the decay time, thus the curvature perturbation evolves gradually. If the curvaton survives long enough, reaches a value with which the dominates the first term, , and the curvaton perturbation is then responsible for the primordial inhomogeneity of the Universe. The large nonGaussianity is possible only when at the decay time is small that is, the energy density of curvaton is subdominant compared to that of radiation. This is because when , the curvaton energy density dominates over the radiation component before decay, then is effectively the curvature perturbation of a single field (curvaton), , and therefore nonGaussianity . We will also see this phenomena in the multifield slowroll inflation later, in Section 3.
2.2. Modulated (P)reheating
After inflation, the energy density in the inflaton field must be transferred into radiation. In the simplest case of adiabatic perturbations, this process does not affect the primordial curvature perturbation on scales which are observable today, because these scale were much larger than the horizon at the time of reheating. However, in a spirit similar to the curvaton model, there may be a subdominant light scalar field present during inflation which modulates the efficiency of reheating. This makes the efficiency of reheating a spatially dependent process. The quasiscale invariant perturbations in this field, which during inflation are an isocurvature perturbation, may be converted into the primordial curvature perturbation during this process. For a review of reheating after inflation, see for example [69, 70].
As a simple illustration of this, in the “old” models of perturbative reheating, the decay rate of the inflaton is given by , where is the strength of the coupling between the inflaton and reheating fields and is the mass of the inflaton. Provided that is much less than the Hubble rate at the end of inflation, so that reheating takes place slowly, the reheating temperature is given by If the coupling strength is a function of the local value of a second scalar field then this will give rise to a perturbation in the decay rate of the inflaton field, and thus in the reheating temperature which is responsible for the density perturbation after reheating. Provided that the field is perturbed, the curvature perturbation can be written as where is a parameter depending on the ratio of to the Hubble expansion at the end of inflation, whose value increases with decreasing and leads to in the limit [33, 71]. Hence, perturbations of the light scalar field can be imprinted into the radiation temperature through the reheating process [71, 72]. In a similar way, the mass of the decaying particle may be modulated [73]. The above equation can be extended to second order, which is required to calculate . In the simple quadratic case that , where and are the homogeneous background part and the perturbation of the field , respectively, the result is [33, 74–76] Hence, we can see that the nonGaussianity can easily be larger than unity in this model by two sources. One is due to the small value of which occurs when the decay rate of the inflation is not much smaller than the Hubble constant at the end of inflation. The other is when is small in which field only controls part of the decay channels of inflaton field.
It is now generally considered that a period of rapid and highly nonlinear preheating preceded the perturbative reheating phase [69]. In this case, one can instead consider modulated preheating, see, for example, [77–79]. A particularly rapid form of preheating, known as instant preheating [80], has attracted more attention in this area, as it is possible to find analytic estimates [81–85]. It is possible to generate the primordial curvature perturbation in these models by having either a weak [81] or a strong [83] symmetry breaking of the twofield potential during inflation which affects the efficiency of instant preheating, or by having two inflaton fields which are coupled with different strengths to the preheat field [82]. However, all of the above models of modulated instant preheating are only allowed, even at the linear level in perturbations, for a small corner of parameter space and even then only for a special choice of initial conditions [85].
2.3. Inhomogeneous End of Inflation
An inhomogeneous phase transition can occur also at the end of inflation between inflationary and noninflationary expansion due to the condition of how inflation ends [34, 86]. In the case of multicomponent inflation, there is a family of inflationary trajectories. If the family of trajectories is not perpendicular to the surface on which inflation ends then there is a possibility that inflation ends on a slice which is not of uniform density and the generation of the curvature perturbation at the end of inflation is expected [34] (This was also discussed in [87–89] using the linear relation between two fields at the end of inflation and the nonGaussianity is transferred from that of the light field which is generated from its nonlinear selfcoupling). In single field inflation, the energy density is determined solely by the single field , and the end of inflation is parameterised by the unique value . If there is another field , then will depend on position through the perturbation . As a result, the change of efolding number from a spacetime slice of uniform energy density just before the end of inflation to a spacetime slice of uniform density just after the end of inflation will have a perturbation . This is the curvature perturbation generated by the end of inflation and can dominate over the contribution from inflation [34].
Using the perturbation of the curvature perturbation generated at the end of inflation is [34]
When dominates the perturbation generated during the inflation, the power spectrum is given by The nonGaussianity can also be generated at the end of inflation since the perturbation at the end of inflation is not required to be Gaussian. Thus, we expect that the observable large nonGaussianity can be generated in this process. From (16) the nonGaussianity is [34] This was applied to the simple example of extended hybrid inflation using sudden end approximation [90, 91].
Recently Sasaki [92], Naruko and Sasaki [93] calculated analytically the curvature perturbation and the nonGaussianity in the multibrid inflation models from horizon exit to the end of inflation considering the general couplings to the waterfall field. In general, we cannot just ignore the curvature perturbation generated during inflation. Furthermore, that is also affected by the end of inflation. A deeper understanding of nonGaussianity both from the evolution during multifield hybrid inflation and effects from the end of inflation is considered by Byrnes et al. [94, 95] which is summarised in Section 3.
3. NonGaussianity during SlowRoll Inflation
It is well known that the single field slowroll inflation with canonical kinetic terms generates a nonlinear parameter of the order of the spectral tilt of the spectrum and thus too small to be observed [13]. On the other hand, in multifield inflationary models the nonadiabatic perturbation may change this conclusion. Furthermore, even within slowroll inflation an observably large nonGaussianity can be generated if certain conditions are satisfied.
Rigopoulos et al. introduced a formalism [96, 97] to deal with nonlinearity based on a system of fully nonlinear equations for long wavelengths and applied it to a twofield inflation model. In the case of twofield quadratic inflation with two massive fields, an analytic calculation is possible with slowroll conditions, and this shows that the nonlinear parameter is small [98, 99]. The numerical calculation confirms the analytical prediction that it is possible to generate a narrow spike of large nonGaussianity while the inflaton trajectory turns a corner, but the nonGaussianity decays quickly after the corner [99, 100]. This spike is due to the temporary jump in the slowroll parameters [101, 102].
Recently, an analysis based on the general analytic formula was done by Byrnes et al. [94, 95], and they showed that it is possible to generate observable large nonGaussianity even during slowroll multifield inflation models and explicitly wrote the conditions as well as concrete examples (There is a claim [103] that the sizeable value of can arise from a loop corrections). In this section, we summarise the general conditions for twofield slowroll inflation to generate a large nonGaussianity and briefly give a specific example. In Section 4 we consider the multifield hybrid inflation model which has been studied in depth, and we include the effects from the end of inflation.
3.1. General Formulas
In the case of a potential which is either sum or product separable, it is possible to compute the curvature perturbation using the formalism and slowroll conditions, and an analytic formula for the nonlinearity parameter can be obtained. The general formula for the nonlinearity parameter was calculated in the case of a separable potential by sum [99], and this was later extended to the noncanonical kinetic terms as well as to the separable potential by product [104]. This has been further generalized to the arbitrary number of fields [105] and to the trispectrum [106].
For a product separable potential, , we can find the number of efoldings analytically in the slowroll limit [107], Then, the power spectrum and the nonlinear parameters can be calculated straightforwardly using the derivatives of efolding number [99, 104, 107]. In the case of two inflatons with canonical kinetic terms, the power spectrum and spectral index are found to be [104] where the slowroll parameters are where is the angle between the adiabatic perturbation and one of the fields and Note that the superscript “*” and “e” denotes that the values are evaluated at horizon exit and at end of inflation, respectively. In the above, and are evaluated at the end of inflation as
The nonlinearity parameter becomes [104] where Similar formulas are found in the case of a sum separable potential [99, 104].
3.2. Conditions for Generating a Large
Using an analytic formula for the nonlinear parameter in the case of a sum or product separable potential, it is possible to generate significant nonGaussianity even during slowroll inflation with Gaussian perturbations at Hubble exit and the general conditions for it can be written explicitly [94].
For the separable potential by product large nonlinear parameter is possible when (there is a symmetric region of large nonGaussianity under the exchange of the two fields). with this condition, the large is given by For large , the substantial increase in is necessary between horizon exit and the end of inflation, which corresponds to the curve of the trajectory in the field space during the slowroll inflation. However, the background trajectory must be almost entirely in the onefield direction.
One specific toy model is the quadratic times exponential potential [94], where the potential is given by With expansion of exponential, this potential can be understood as the quadratic chaotic inflation model which has a coupling to another light scalar field. For this potential, considering the condition for large nonGaussianity, (26), large is generated when the at horizon exit is small. One example is found to give with for and .
For a sum separable potential, we can find similar conditions for generating a large [94].
4. Hybrid Inflation with Two Inflaton Fields
We consider a model of two field hybrid inflation, whose potential is given by which is vacuum dominated, that is, which satisfies and . It is in this regime that the two ways of writing the potential given above are equivalent (at leading order in slow roll), so we can treat the potential as being both sum and product separable. We assume that inflation ends abruptly by a waterfall field which is heavy during inflation and hence does not affect the dynamics during inflation. First, we calculate observables during slowroll inflation. We will consider the full potential including the waterfall field in Section 4.2, which incorporate the effects from the end of inflation considered in Section 2.3. We will see that this can lead to a change in observables on the surface where the waterfall field is destabilised.
In the vacuumdominated regime, the slowroll solutions are where “*” denotes the value at the horizon exit. Throughout this section, whenever we write a quantity without making it explicit at which time it should be evaluated, we mean the equation to be valid at any time foldings after Hubble exit and while slow roll is valid. Generally, we will be interested in quantities at the end of inflation, in which case we take .
The slowroll parameters are We note that the dominant slowroll parameters and are constants during inflation in the vacuum dominated regime and that they are much larger than the slowroll parameters and throughout inflation.
From the previous section, large nonGaussianity can be realised in either of two regions Since the two regions are symmetrical [94] (before specifying the values of and ), in the rest of this section, we will focus on the second region. In this region where , is fulfilled by the condition in other words, This implies three inequalities on Note that in this region from (30), we require so that grows significantly during inflation.
4.1. Simplified Formula for the Observables When Is Large
We can substantially simplify all of the above formula in the case where is large. We define the quantity In the region, we are considering where is large, this is approximately given by the initial and final angles of the background trajectory with different exponents
In the case of large nonGaussianity it follows that
The first condition in (35) implies that We, therefore, require a very small value of in order to have a large nonGaussianity. While this may be a fine tuning, we comment that requiring a large ratio of the initial field values is common in models where the isocurvature perturbation generates a significant part of the primordial adiabatic perturbation, see the discussion in the conclusion of [85]. If the inflaton perturbations are neglected a priori, such as in the pure (i.e., not mixed) curvaton scenario, this remains implicitly true. For an explicit discussion of this, in the simple case that both the inflaton and curvaton fields have a quadratic potential, see [108].
The sign of is determined by the sign of . The amplitude of depends exponentially on the difference of the slowroll parameters, , which we require to be positive to be in the branch of large nonGaussianity where , while the spectral index depends on a weighted sum of the slowroll parameters, so it is possible to have a large nonGaussianity and a scale invariant spectrum. However, it is not possible to have a large and positive and a red spectrum of perturbations. We will see in Section 4.2.2 that by including the effect of the waterfall field this conclusion may change, depending on the values of the coupling constants between the two inflaton fields and the waterfall field.
In Table 1, we give some explicit examples of values of and which lead to a large nonGaussianity. Using (4), we also calculate the spectral index. The first example in Table 1 shows that it is possible to have and a scale invariant spectrum. We also see that it is possible to generate a large nonGaussianity during slow roll with and both positive or both negative, or when one is positive and the other negative corresponding to a saddle point. The results for this model were verified using a novel calculational method of momentum transport equations in [109].

4.2. Effect of the Waterfall Field and Further Evolution after Inflation
In this section, we include the effects of the waterfall field which is required to end hybrid inflation. Inflation ends when the waterfall field is destabilised that is, when its effective mass becomes negative. During inflation, the waterfall field is heavy, and it is trapped with a vacuum expectation value of zero, so we can neglect it during inflation. The end of inflation occurs when the effective mass of the waterfall field is zero, which occurs on a hypersurface defined in general by [92, 93] which is realised by the potential , defined by (29), where is given by Here, () is the coupling between the () field and is the waterfall field with selfcoupling . In general, the hypersurface defined by this end condition is not a surface of uniform energy density.
As discussed earlier, this is an example of a model with an inhomogeneous end of inflation, that is, where inflation ends at slightly different times in different places. It has also been shown for the hybrid potential we are considering that this can be used to generate a large amount of nonGaussianity, for certain parameters values and fine tuning of the parameters [90, 93]. However, these papers concern the large nonGaussianity generated at the end of inflation rather than during slowroll inflation, by having a very large ratio of couplings . Here, we consider the case where and have the same order of magnitude with in Section 4.2.1 and with in Section 4.2.2.
4.2.1.
In this case, we have chosen the coupling constants (which can satisfy and/or ) such that the surface where the waterfall field is destabilised corresponds to a surface of uniform energy density. This is because the end condition can be rewritten as . In this case, the value of all observable quantities such as the power spectrum and nonGaussianity are the same as those we calculated previously which were valid at the final hypersurface of uniform energy density during inflation.
4.2.2.
In this case, the end of inflation given by the condition in (43) does not occur on a uniform energy density hypersurface [93]. We will show how the nonGaussianity is modified by the condition at the end of inflation in this example. In general, we expect there to be some modification to nonGaussianity from the end of inflation, except in the special case we considered in Section 4.2.1. We have checked in [95] that the correction from the extra expansion which occurs from the surface on which inflation ends up to a surface of uniform energy density is small, and therefore one can still use the formalism in this case.
In this case, the power spectrum and in the limit of large nonGaussianity are [93] We can see that the observables at the end of inflation are changed by the additional ratio of before . Furthermore, has an additional factor of .
In Table 2, we show the values of , and with end condition for the same parameter values that we used in Table 1, where the inflation ends on the uniform energy density hypersurface. The first two examples show that if , then the observables are unchanged for two different end conditions except that the sign of is switched. The second example in the table shows that in this case it is possible to have a red spectral index and a positive value of . For many values of the initial parameters when , the magnitude of decreases compared to Table 1, but the reverse can also happen, an example of this where grows by more than an order of magnitude is shown in the final row of Tables 1 and 2.

4.2.3. Further Evolution after Inflation
So far, we have assumed a quick transition to the radiation epoch at the end of inflation, thereby neglecting the dynamics of the waterfall field. However, if we consider the role of the waterfall field, then after the waterfall field is destabilised, there may be a further evolution of the primordial curvature perturbation, which will lead to a change of the observable parameters. This applies to any model with an inhomogeneous end of inflation, since there are isocurvature perturbations still present after the waterfall field is destabilised and inflation has ended. Further evolution will depend on the details of reheating in a model dependent way. To the best of our knowledge, this issue has not been considered in depth in any paper. If we assume an instantaneous transition to radiation domination (so a completely efficient and immediate decay of the waterfall and inflaton fields), then there will be no further change to the observables as we have argued in the previous section. However, this is clearly an idealised case.
In the special case where the waterfall field is also light during inflation, Barnaby and Cline [110] have shown there is the possibility of generating a large nonGaussianity during preheating for certain parameter values. This is possible even if there is only one inflaton field and the waterfall field present. However, in this case, inflation does not end abruptly when the waterfall field is destabilised so this is not the scenario we have considered in this paper. A recent claim that even a heavy waterfall field may lead to a scale invariant local nonGaussianity has been withdrawn [111].
5. MultipleField Inflation without Slow Roll
In this section, we demonstrate a new method that provides, for certain classes of models, analytical expressions for valid in regimes beyond a slowroll approximation [112]. This method is based on the firstorder HamiltonJacobi formalism developed by Salopek and Bond [113], which allows us to express inflationary observables in the multifield case, without having to focus on a slowroll regime (see [114] for a similar application of this formalism to the singlefield case).
The main idea on which our arguments are based is to focus on inflationary multifield trajectories in which the Hubble rate, and not the potential, is separable. This approach allows us to analytically study cases where the nonGaussian parameter becomes large, in regimes in which the slowroll parameters are enhanced after Hubble exit, but before inflation ends. In particular, we provide analytical equations that express the nonlinearity parameter , in terms of quantities that generalise the slowroll parameters during inflation. Using this method, we demonstrate in the next subsection an exact solution of multifield inflation which can give rise to a large nonGaussianity due to a strong break down in slow roll shortly before inflation ends.
The firstorder HamiltonJacobi equations of motion are
We concentrate on solutions satisfying the following Ansatz for the Hubble parameter that is, we demand that it can be split as a sum (hence, we follow an analysis related to [99]. In an analogous way, one could also consider a situation in which the Hubble parameter splits as a product of singlefield pieces [104]. The formula's in this section were extended to an arbitrary number of fields with a sum separable Hubble parameter in [115]) of two pieces, each one depending on a single field. Notice that this is different with respect to the requirement of separable potentials usually done in the literature and earlier in this paper.
It is convenient to define the following quantities: and . Although their definition resembles the corresponding one for the usual slowroll parameters and , they do not coincide with them when taking a slow roll limit (it is nevertheless simple to work out the relation with the slow roll parameters, defined by (21) and (22). In a slowroll regime, one finds ). We assume that the quantities and are much smaller than unity at Hubble exit , in order that we can use the formalism. During inflation, by definition, we have to ensure that the quantity . The quantities can, however, become much larger than unity during inflation.
Using similar techniques to those applied to a separable potential, one can calculate the spectral index and , the details were given in [112] and the results are where the new symbols are defined by
We reiterate that the formula for is exact (apart from neglecting a slowroll suppressed contribution due to the nonGaussianity of the fields at Hubble exit) and is not based on a slowroll expansion. Although and are necessarily small, the quantity is not suppressed by these parameters and can assume large values during inflation, enhancing . We note in agreement with [99] that if one of the fields has reached a minimum so or at the end of inflation then and the nonGaussianity at the end of inflation will be very small. Therefore, any model of inflation with a separable potential or separable Hubble factor with a large nonGaussianity present at the end of inflation must have both fields still evolving, and therefore the presence of isocurvature modes. It would, therefore, also be interesting to study the evolution of the perturbations after inflation, to see if this leads to an important change in the observables [116].
5.1. Exact Solution
Very few exact solutions in multiplefield inflation are known [117]. Here, we present an exact solution which can give rise to a very large nonGaussianity at the end of inflation. A potential with a similar form may be motivated in string theory, in the context of Kähler moduli inflation [118–125].
The potential we consider is [112] where the parameters and satisfy
The HamiltonJacobi equations have the following exact solution for and the fields: where we have defined , is cosmic time, and we have set . The overall factor to the potential can be freely chosen so that the amplitude of the scalar power spectrum matches the observed amplitude of perturbations in the CMB. The scale factor results Notice that the solution becomes singular at late times, when the scale factor vanishes and the field values diverge. This singularity occurs well after inflation ends, and we will not need to discuss it in our analysis. From the relations we notice that in this example and can become much larger than unity at the end of inflation if and/or are much greater than one. This corresponds to a break down in slow roll, although remains smaller than unity during the inflationary era by definition.
As a simple, concrete example of parameter choice which gives rise to a large nonGaussianity, we choose a regime in which the parameters and are both large, let us say larger than some quantity . We note from (56) that we are, therefore, required to have and . In this case, the potential does not have a minimum, but inflation still ends through growing larger than unity, and we can trust our results in this regime. The potential would need modifications which apply after inflation in order for reheating to take place and these modifications may provide a minimum for the potential. We parameterise the values of the quantities and at the end of inflation as where the final equality follows from . We assume that the quantities and are not too big. Namely, they satisfy the inequality . This implies that . We choose , , such that we can write This fixes the initial values for the fields and , to the values
The conditions (60) imply Since and are much smaller than , we expect . We hence have the simple relations From (52), we find So, we have a red spectral index in agreement with present day observations [126] and in [112] it was also shown that the tensortoscalar ratio for this model is negligible.
When evaluated at the end of inflation, we find We stress that this formula provide only the dominant contributions to . It is valid in the case , and .
As an explicit case, we take and the initial conditions to satisfy (62) with . Then, independently of the values of and , we find from the simplified formula (66), and from the full formula (53). See Figures 1 and 2. Notice that the results for differ from each other by quantities of order as expected by the approximations we have made. At the end of inflation, the parameters are , and this shows that the slowroll approximation has been significantly broken, (it is nevertheless simple to work out the relation with the slow roll parameters, defined by (21) and (22). In a slowroll regime, one finds ). From Figure 2, one can see that the trajectory is straight for much of inflation but it turn near the end of inflation (during the last efolding before inflation ends), and it is during this time that grows larger than unity.
(a)
(b)
Notice that our requirements of final values for the quantities and (both much bigger than ) imposes finetuning constraints on the initial conditions, since at leading order in the values for and must coincide (see (62) and recall that ).
We stress that the enhancement of nonGaussianity occurs towards the end of inflation. What happens just after inflation is a modeldependent issue; we cannot address this question within the approximations used in this concrete model. For our choice of parameters, we notice that is still increasing at the end of inflation, see Figure 1, but for other choices it may start to decrease before inflation ends, see [115]. We stress that in the regime where the slowroll parameters will necessarily become much greater than unity by the end of inflation, which may correspond to : this is one reason by which can become large. Our formalism is at least in principle suitable to study the evolution of nonGaussianity after inflation, when the parameter becomes larger than unity (although we restate that the specific potential being considered here anyway needs to be modified after inflation ends).
6. Higher Order NonGaussian Observables
NonGaussianity is most popularly parameterised in terms of one nonlinearity parameter, . There are several different 's used in the literature which parameterise different shape dependences of the bispectrum [41, 42], the most popular being the local model discussed in this paper and the socalled equilateral model which can arise from models of inflation with noncanonical kinetic terms (a popular example is DBI inflation [15–25]). But can we learn more than one number from an observation of nonGaussianity? And if is detected how can we hope to distinguish between the models which can generate this? Fortunately, observations of nonGaussianity have the possibility of teaching us much more than the value of one parameter. Two examples of further nonGaussian observables are a scale dependence of and the trispectrum.
6.1. Trispectrum
The four point function of the primordial curvature perturbation is defined by which using the formalism, and assuming that the fields have a Gaussian distribution at Hubble exit, is given by where , and the trispectrum nonlinearity parameters can be calculated using [98, 106, 127] Hence, we see that the trispectrum depends on two nonlinearity parameters (as opposed to one, , for the bispectrum), and they may be observationally distinguishable since they are prefactors of terms with different shape dependences (68). The current observational bound on the local type of the bispectrum from seven years of WMAP data is at the level [2]. Recently, there has been a first constraint on both and , which came from using WMAP5 data, with the bounds and at confidence [128]. There have been two other observational constraints on the trispectrum through , setting . The bounds, which in both cases are roughly 10^{5}–10^{6}, come from large scale structure [129], and the CMB [130]. If there is no detection of nonGaussianity it is expected that with Planck data the bounds will be reduced to about , and at the level and future observations may become even tighter [131–135]. Note that the expected future constraint on is about two orders of magnitude weaker than that on [135]. We will see that it is also possible for some models and parameter ranges that the first observational signature will come through the trispectrum rather than the bispectrum.
6.1.1. Trispectrum in TwoField Hybrid Inflation
In the regime where and are greater than unity, they are given by We see that is subdominant to and hence will not provide a competitive observational signature. It follows from (71) that , so may be large and provide an extra observable parameter for this model. This inequality between and is true in general [75], and equality is reached whenever a single field direction during inflation generates the primordial curvature perturbation. However, it is usually assumed that since both arise from second derivatives in the formalism. In fact, for our model it is possible to have a small (and hence also a small ) but a large and potentially observable . For this, we require that , although in practice if we make it too small it may no longer be possible to satisfy a constraint on a minimum possible field velocity consistent with a classical slowroll trajectory, as discussed in [95] (see also [136] and a discussion which reaches a different conclusion is given in [137]). In the final example in Table 1, we give an explicit example of parameter values which give rise to an which is probably too small to be detected with Planck but with a very large trispectrum through that should be detectable at a high significance. For another example with but , see [76]. In contrast, it has been shown in several papers [127, 138–142] that in the curvaton scenario where the curvaton has a nonquadratic potential it is possible to realise while is small with some tuning of parameters. This is also possible in the exact solution which we presented in Section 5 and we consider this next.
6.1.2. Trispectrum in the Exact Solution
In this regime, where and , it is also possible to give compact expressions for the trispectrum (4point function) nonlinearity parameters, in terms of as The complete result was given in [115]. Hence, both of the trispectrum nonlinearity parameters are generally large whenever is. We note that if then from (60) , so the trispectrum through will give the dominant signal of nonGaussianity through a large, negative .
6.2. Scale Dependence of
In its simplest form, the local form of defined by (1) is a constant parameter, independent of both position and scale. However, in realistic models is likely to be mildly scaledependent. This may happen in two ways. In general, singlefield models (such as the curvaton scenario) where the scalar field which generates the primordial curvature perturbation has a nonquadratic potential the nonlinearities this generates will give rise to scale dependence of . Alternatively, even in models where all of the fields have a quadratic potential; if the primordial curvature perturbation has contributions from more than one field, and the fields do not all have the same mass, then will again have a scale dependence. This is because the correlation between the first and second order terms of , which the bispectrum depends on, will become scaledependent. This is indeed what happens in the twofield hybrid model presented earlier. For details about a scale dependence of local , see Byrnes et al. [143].
We define a second observable parameter derived from the bispectrum which is analogous to the scale dependence of the power spectrum. There is a subtlety here, which is that in general may depend on three independent parameters, , and . However, it was shown in [143] that provided one takes the derivative while keeping the ratio of the three vectors fixed then is independent of the shape of the triangle described by the three vectors, which makes this a well defined quantity. Observational prospects for this quantity were considered in [144], who showed that the Planck satellite is sensitive to , assuming a fiducial value of . This observational sensitivity to is about a factor of two larger than the current preferred value of the power spectrums spectral index and may therefore provide an interesting extra constraint on nonGaussian models. The scale dependence of an equilateral form of has also been considered from both a theoretical and observational perspective, see for example [144–147].
In the example of twofield hybrid inflation, has a scale dependence both because of the exponential term in , (41), and because will vary through the change of the initial value of . We find Using this we find from (41) that In the case that we include the effect from the surface where the waterfall field is destabilised and , we find from (48) that For both cases, the spectral index of satisfies for any value of and hence will be smaller on small scales.
Because we require a relatively large value of for our model to generate a large nonGaussianity it is quite possible for our model to generate a relatively significant scale dependence of . However, the amount also depends on , and when this is large, then the field is almost solely responsible for generating at both first and second order and is suppressed. We can also see in agreement with the statement at the beginning of this subsection that in this case, if the mass of the two fields are equal, then the two fields have the same scale dependence and .
We note that this is in contrast to the large nonGaussianity from an inhomogeneous end of inflation found in [93]. In the specific cases, they considered to generate a large nonGaussianity the nonGaussianity was generated purely at the end of inflation and is scaleindependent. In detail, we see from and in [93] that their formulas for does not depend on or on any quantities evaluated at Hubble exit. This is also in contrast to the exact solution considered in Section 5.1. Our expression for in (66) depends on the initial values through and , and this dependence drops out at leading order in . Hence, is independent of the number of foldings and scaleindependent.
7. Conclusions
We have reviewed various models which can generate a large local nonGaussianity. A feature shared by all of these models is that they have more than one light scalar field present during inflation. This extra degree of freedom generates an isocurvature perturbation which is at least partially converted into the primordial curvature perturbation after horizon exit of the modes which are observable today. In the curvaton and modulated reheating scenarios, this conversion occurs after the end of inflation, while in the inhomogeneous end of inflation scenario, this conversion occurs on the nonuniform energy density hypersurface on which inflation ends. For these three scenarios, the light field which generates the primordial curvature perturbation after or at the end of inflation can be treated as a test field which does not affect the inflationary dynamics.
Our main focus has been on models in which a large nonGaussianity is generated during inflation. This can occur even within slowroll inflation for certain potentials and certain trajectories. We have shown, at least in the case of a separable potential, that the trajectory is required to be almost entirely along the direction of one field but that the orthogonal field must become more important towards the end of inflation, and hence the inflationary trajectory must curve. In absolute terms, the change to the angle of the background trajectory is small (compared to a trajectory which turns by a right angle during inflation), but in relative terms it must grow by at least an order of magnitude. This is in contrast to the previous three scenarios.
We have reviewed twofield hybrid inflation as an explicit model of a separable potential where the conditions required to generate a large nonGaussianity can be satisfied. The conditions can be satisfied for any possible combination of positive and negative parameters, so the potential can be bowlshaped, a hilltop, or have a saddle point. The main conditions which must be satisfied is that the difference of the two parameters must not be too small, , and the value of the field must be very subdominant to that of the field initially (or vice versa). In general, but depending on the coupling constants between the two inflaton fields and the waterfall field, there is a change to observables at the end of inflation, due to the fact that the surface on which the waterfall field is destabilised and inflation ends might not be a surface of uniform energy density. This effect is responsible for the inhomogeneous end of inflation scenario. It is then a model, dependent question whether there will be further evolution to the observables during reheating in this model, this deserves further attention.
One similarity that this hybrid inflation model has together with the quadratic curvaton scenario is that in both cases the initially subdominant (approximately isocurvature) field has the ratio approximately constant and the field fluctuations do not become more nonGaussian with time. However, the effect of this light field on the primordial curvature perturbation grows, during inflation in the hybrid scenario and before the curvaton decay in the curvaton scenario. It is this nonlinear transfer between the field fluctuation and , described by the