Dissipative length scale estimates for turbulent flows - a Wiener algebra approach
In this paper, a lower bound estimate on the uniform radius of spatial analyticity is established for solutions to the incompressible, forced Navier-Stokes system on an -torus. This estimate improves or matches previously known estimates provided that certain bounds on the initial data are satisfied. It is argued that for 2D or 3D turbulent flows, the initial data is guaranteed to satisfy these hypothesized bounds on a significant portion of the 2D global attractor or the 3D weak attractor. In these scenarios, the estimate obtained for 3D generalizes and improves upon that of , while in 2D, the estimate matches the best known one found in . A key feature in the approach taken here, is the choice of the Wiener algebra as the phase space, i.e. the Banach algebra of functions with absolutely convergent Fourier series, whose structure is suitable for the use of the so-called Gevrey norms.
Key words and phrases:Navier-Stokes equations, turbulence, radius of analyticity
2010 Mathematics Subject Classification:35Q30, 76D05, 76F02, 76N10
A. Biswas]firstname.lastname@example.org M. S. Jolly]email@example.com V. Martinez]firstname.lastname@example.org E. S. Titi] email@example.com
The conventional theory of turbulence posits the existence of certain universal length scales of paramount importance. For instance, according to Kolmogorov, there exists a dissipation length scale, , beyond which the viscous effects dominate the nonlinear coupling. This length scale can be characterized by the exponential decay of the energy density. Consequently, one expects the dissipation wave-number, , to majorize the inertial range where energy consumption is largely governed by the nonlinear effects and dissipation can be ignored.
In [13, 9] it is shown that as characterized by Gevrey norms, the (uniform) radius of spatial analyticity, here denoted , provides a lower bound for the dissipation length scale, i.e., . The space analyticity radius has been well-studied over the years, especially after the pioneering work of Foias and Temam in , where they presented a novel Gevrey norm approach to establish analyticity of solutions to NSE in both space and time. An advantage of this approach is that it avoids having to make cumbersome recursive estimates on derivatives. Consequently, it has become a standard tool in estimating the analyticity radius for various equations (cf. [12, 33, 32, 29, 3, 2, 27, 28]).
Kolmogorov’s theory for 3D turbulence asserts that
where is viscosity and is the mean energy dissipation rate per unit mass.
For 3D decaying turbulence, it is shown in  that
where is as in (1.1), except that the energy dissipation rate is a supremum in time rather than an averaged quantity (see (3.11), (3.14)). The more significant discrepancy is a power of 4 versus a power of 1 in (1.1). Our improvement is done under the 2/3-power law assumption (3.16) on the energy spectrum for a forced, turbulent flow, by means of an ensemble average with respect to an invariant measure. It is valid on a portion of the attractor (weak in the 3D case); the significance of which is quantified in terms of this measure. Ultimately, we conclude that
holds with probability , where the suppressed constant in the inequality tends to as . Similarly, a heuristic scaling argument by Kraichnan for 2D turbulence leads to
where is the mean enstrophy dissipation rate per unit mass. We show that if the 2D power law (3.26) for the energy spectrum holds, then
up to a logarithm in .
These improved estimates actually follow from more general bounds on the radius of analyticity which require the solution to satisfy a certain “smallness” condition. Those conditions are met under the power law assumptions, when averaged with respect to an invariant measure. Kukavica  achieved the same bound in 2D up to a logarithmic correction on all of the attractor using complex analytic techniques, interpolating between norms of the initial data and the complexified solution, and invoking the theory of singular integrals.
The approach in  was actually a modification of the approach in , where it was shown that . It is interesting to ask if these estimates can be obtained by working exclusively in frequency-space using Fourier techniques, rather than in physical space with the norm. Indeed, this is an impetus of our work.
The technique applied here combines the use of Gevrey norms with the semigroup approach of Weissler . Motivated by recent developments, we work over a subspace of the Wiener algebra, whose norm is a Sobolev-Gevrey-type norm in (see (2.11)). This norm and approach was applied in  to study spatial analyticity and Gevrey regularity of solutions to the NSE. However, the resulting estimate on the spatial radius of analyticity was not optimal for large data. This approach is refined here to obtain a sharper estimate for such data. The advantage of working in the Wiener algebra, , i.e. the Banach algebra of functions whose Fourier series converge absolutely, was explored in , where a sharp estimate on the radius of analyticity was obtained, for instance, for real steady states of the nonlinear Schrödinger equations. More recently, these -based Gevrey norms were also applied to the Szegö equation in  and the quasi-linear wave equation in . In , an essentially sharp estimate on the radius is obtained there as well. While these works used energy-like approaches, the effectiveness and robustness of as a working space to study analyticity has become increasingly clear.
There are several advantages to our approach. First, our method is quite elementary. Since is embedded in , we essentially recover the results of  and  without resorting to complex-analytic techniques and the theory of singular integrals, while furthermore allowing for rougher initial data. Secondly, this approach also applies to the case , thereby unifying the results of , , , and  . Thirdly, no logarithmic corrections appear in our estimates initially; they only appear when specializing to the context of 3D or 2D turbulence (see (3.1.2)). Finally, the method is rather robust and applies to a wide class of active and passive scalar equations with dissipation, including the quasigeostrophic (QG) equations. Note that in the case of QG with supercritical dissipation, the method will only accommodate subanalytic Gevrey regularity (see ).
The Navier-Stokes system in for is given by
where and are given, and and are unknown. We assume that are all -periodic and mean-zero, and that is divergence-free.
where , such that , and , where is the Helmholtz-Leray orthogonal projection, i.e. projection onto divergence-free vector fields,
Recall also that the mean zero condition forces for all . The bilinear term has Fourier coefficients given by
Note that will denote the sequence .
and also that the following basic convolution estimate holds
Since we will be working with (2.2), we choose an appropriate sequence space as our ambient space. Define
where . For define
and denotes an element of . Observe that when , the norm on agrees with that on the Wiener algebra, i.e.
where is the continuous function whose Fourier coefficients are given by . In fact, we have , for all .
For , we define the (analytic) Gevrey norm of by
for . Observe that has the physical dimension of length.
For a time-dependent sequence such that , for all , we define the (analytic) Gevrey norm of by
where is increasing and sublinear, i.e. for all . Observe that
for all and , where if and otherwise.
If , then admits an analytic extension on ;
If has an analytic extension on , then for all .
In particular, if a function has finite Gevrey norm, then the Fourier modes decay exponentially. Indeed, if , then
If is analytic, then we define
to be the the maximal (uniform) radius of spatial analyticity of . Moreover, due to (2.14) we have .
For convenience, we adopt the following conventions for the rest of the paper.
We will usually write simply as , which is the function whose Fourier series have modes , for .
By or , or when the context is clear, simply , we shall mean the time-dependent sequence , unless otherwise specified.
We will use to suppress extraneous absolute constants or physical parameters. In some instances, the dependence of these constants will be indicated as subscripts on .
We will also use the notation to denote that the two-sided relation and holds.
For and , we define
For any dimension , the Grashof number is defined as
Observe that and are dimensionless. One can show that when is time-independent and has only finitely many modes, i.e. , where
then is comparable to up to a constant depending on only , a fixed parameter , and , where satisfies
see Proposition 23 in Appendix.
Now suppose that data and are given such that . Let be the Stokes operator, , where is defined as in (2.3). Then the heat kernel, , is the Fourier multiplier defined by
or equivalently, . We will use two notions of solutions to (2.2).
For , a mild solution to (2.2) is any function such that
for all , and
for all .
For , a weak solution to (2.2) is any function such that
for all and a.e. and
holds for all and a.e. .
Finally, we define the regularity that we ultimately seek to establish.
A mild or weak solution of (2.2) is Gevrey regular if there exists and sublinear such that
3. Main Theorems
We first state a result for a general force.
Let and and be as defined in (2.18). Suppose that and are given such that . Then for some , there exists a mild solution to (2.2), which is also a Gevrey regular weak solution, with radius of analyticity at time satisfying
where . Moreover, there exists a constant such that if , then one may take . In this case, the solution exists for all and the radius of analyticity at time satisfies
In the case where the forcing is time-independent and has finitely many modes, we can express the estimate on the radius of analyticity in terms of the Grashof number, provided a “smallness” condition on the solution holds.
Suppose that is time-independent and satisfies . If
then for some , there exists a unique weak solution to (2.1) such that is Gevrey regular and the radius of analyticity at time satisfies
The following estimate is not as sharp, but holds under a weaker “smallness” condition.
Suppose that is time-independent and satisfies . If
where with periodic boundary conditions, is the Stokes operator, then for some , there exists a weak solution to (2.1) such that is Gevrey regular and the radius of analyticity at time satisfies
which is less sharp than the corresponding estimate in (3.1) when is large.
One should also note that if is too small, then the global attractor in 2D becomes trivial (cf [6, 30]). Physically, this corresponds to the case of decaying turbulence. Nevertheless, if is sufficiently small, then is allowed, in which case the solution exists globally in time with radius that grows without bound in time as .
Uniqueness of weak solutions to (2.1) is guaranteed in two-dimensions, but in 3D is still an open question. There are, however, cases where the uniqueness is guaranteed in any dimension (see  pp. 298-99). In particular, as long as , the solution of Theorem 3 is unique in the class of weak solutions.
where represents the radius of analyticity at some time strictly less than the maximal time of existence. The constant here can be explicitly identified as , where is the nontrivial solution to
Note that (3.8) is precisley the estimate in (3.1) (up to an absolute constant). The energy approach, however, encounters technical difficulties when one includes forcing on infinitely many scales. The reader is referred to  for additional details.
In , the estimates are also done in for . In particular, when , the result of  is generalized to include forcing on all scales, and the estimate on the radius is the same as the one derived there (up to an absolute constant). One can make an argument similar to the one presented in Section 3.1 that would justify the corresponding assumption on the initial data, but working on the 3D weak attractor. For background on the weak attractor, see  or .
Finally, the techniques used to prove Theorem 4 apply equally well to the vorticity formulation of Navier-Stokes, the case of fractional dissipation, and a wide class of active and passive scalar equations, including 2D dissipative QG equations, (see ). These techniques also apply to the case (see ). For more results on the subcritical QG, see for instance , where analyticity is established for arbitrary initial data in , or , where a local smoothing effect is exploited to establish analyticity, or , where analytic Gevrey regularity is established for several other equations as well. For results on the analyticity of solutions for critical QG equations, see  and . For results on the regularity of passive scalar equations see  or . The classical Hilbert space techniques of  have also been successfully applied to the Euler equations (see  and ).
3.1. Application to Turbulent Flows
In this subsection, we show how our results in Theorems 4, 5 improves the known estimates for for turbulent flows. While their “smallness” assumptions may not hold on all of the 2D global (3D weak) attractor, in the context of turbulence, one can expect these conditions to hold on average, in a precise sense.
The statistical theory of turbulence concerns relations between quantities that are averaged, either with respect to time or over an ensemble of flows, e.g. results from repeated experiments. It is remarkable that these two seemingly different approaches are in fact related.
The mathematical equivalent of a large time average is rigorously expressed in terms of Banach limits. Following , define the space by
Let be a real-valued weakly continuous function on . Then for any weak solution of (2.2) on , there exists a probability measure for which
where is a Hahn-Banach extension of the classical limit. The measure is called a time-average measure of . Note that neither nor are unique. The use of surmounts the technical difficulty that the limit in the usual sense may not exist. If is weak solution to the 2D NSE, then by regularity of such solutions, one can work in the strong topology on . Moreover, by uniqueness, one can show that is in fact invariant with respect to the corresponding semigroup, i.e. for all , for all measurable sets . Thus, a time average measure is also a so-called stationary statistical solution of the NSE. For a more detailed background see .
We now specialize to the cases of 3D and 2D turbulence, and interpret the main theorems in those settings.
3.1.1. 3D Turbulence
The mean energy dissipation rate per unit mass is defined as
In 3D, Kolomogorov argued that because one can ignore nonlinear effects in the dissipation range, the length scale indicating where dissipation is the dominant effect should depend solely on and . By a simple dimensional argument, one then arrives at
In other words, according to Kolmogorov, for turbulent flows in 3D, with given in (3.12). We will now describe the best known rigorous result in this direction.
In , the radius of analyticity was estimated in terms of as
represents the largest instantaneous energy dissipation rate (per unit mass) up to time , and is the maximal time of existence of a regular solution. A heuristic argument is given to support as in , then (3.13) becomes
It is not presently known if remains finite beyond . Hence, it is not possible to obtain an estimate of the smallest length scale for an arbitrary weak solution. In fact, it is not possible to extend these estimates on the weak attractor either since it is not known whether or not a trajectory, i.e. a weak solution defined for all , is regular. However, it is well-accepted that statements regarding length scales in turbulence actually concern “averages” and not specific trajectories (cf. [14, 16, 18, 1], or [17, 19] for introductory approaches). Indeed, this is the thrust of our current discussion.
In addition to the dissipation range and wave number, another basic tenet in the Kolmogorov theory of turbulence is the so-called power law for the energy spectrum. More specifically, let denote the wave number in which energy is injected into the flow, i.e., . Denote the Kolmogorov wave-number . Then the range of wave-numbers is known as the inertial range in which the effect of viscosity is negligible. The nonlinear (inertial) term simply transfers the energy injected into the flow through the inertial range at a rate of . Moreover, defining the quantity
the well-celebrated Kolmogorov’s power law asserts that a turbulent flow must satisfy the relation
Additionally, it is also known that if the Grashof number is sufficiently small, then the flow is not turbulent and the attractor in this case consists of only one point. In view of this discussion, we define a flow to be turbulent if the Kolmogorov power law holds and the Grashof number is sufficiently large, i.e.
It is shown in  that for such a flow one necessarily has the bounds
The following is the main result of this section which improves upon the estimate in  for 3D turbulent flows.
Let be a time-average measure for a 3D turbulent flow and let . There exists a set with such that
Recall that Theorem 5 ensures that
provided that the initial data satisfies
First, observe that by Proposition 25 with , one has the inequality
Let and define the following sets
This combined with (3.22) implies that
Then Theorem 5 gives
where suppresses a constant which tends to as . Finally, observe that (3.19) implies that , so that . Therefore
where denotes the radius of analyticity of at time .
In particular, we have just shown that for any , the radius of analyticity for the corresponding solution at time is bounded below by
provided that we are in the turbulent scenario described above. ∎
3.1.2. 2D Turbulence
In the Kraichnan theory of 2D turbulence enstrophy is also dissipated, and it does so at a mean rate per unit mass given by
Two key wave numbers are
where is the Stokes operator.
It is shown in , that if the well-recognized power law
holds on over the inertial range and if
This is to say that on average is of order on the global attractor. As in the 3D case, we can make this precise in terms of probabilities.
First, observe that by the “time-averaged” Brézis-Gallouët inequality (see Proposition 24)
As before, Chebyshev’s inequality then implies
where the constant inside depends only on , , and logarithms of . Since by (3.29)
we have the following
Let be a time-invariant measure for a 2D turbulent flow and let . There exists a set with such that
There are also 3D versions of a time-averaged Brézis-Gallouët inequality, i.e. Proposition 24, which accomodate the endpoint cases of the Agmon-type inequality in Proposition 25, namely, and . However, neither of these cases fit within our discussion. Indeed, in the case , one must have some control over the quantity , which is not presently known. On the other hand, although we do have control over the quantity in 3D, in this case the Brézis-Gallouët inequality will only provide an estimate for the quantity , which lies outside of the range allowed by Theorem 20. Let us lastly note that if one could control , at least on average, then one could argue as before and apply Theorem 20 to obtain the estimate .
4. Outline of Proofs of Main Theorems
Following , our approach is to use a contraction mapping argument. Fix , , and . Define the spaces
where are equipped with the norms
and . Then are Banach spaces with continuously. Observe moreover that these norms are dimensionless.
By the Duhamel principle, the solution that we seek will be a fixed point of the operator defined by
In particular, we establish the existence of such a function in the closed subset given by
for some , which satisifes . To do so, we will invoke the following existence theorem whose proof can be found in .
Suppose that and that for some . If and whenever and , for given by either
then there exists a unique such that