Current-sensorless robust sliding mode control for the DC-DC boost converter

1.   Introduction

In this paper, we are concerned with the sharp decay rates of solutions to the Cauchy problem for the isentropic Navier-Stokes equations:

which governs the motion of a isentropic compressible viscous fluid. The unknown functions $\rho$ and $u$ represent the density and velocity of the fluid respectively. The pressure $p = p(\rho)$ is a smooth function in a neighborhood of a positive constant $\bar \rho$ s.t. $p'(\bar \rho)>0$. $T$ is the viscosity stress tensor given by $T = \mu({\nabla} u+({\nabla} u)^t)+\nu({\mathop{{\rm{div}}}\nolimits} u)I$ with $I$ the identity matrix. We assume that the constant viscosity coefficients $\mu>0$ and $\nu$ satisfy $\nu+\frac23 \mu>0$. Throughout this article, by optimal time decay rate, we refer to the best possible decay rate in upper bound as many literatures, and the sharp time decay rate includes the best possible upper and lower bounds.

Using the classical spectral method, the optimal time decay rate (upper bound) of the linearized equations of the isentropic Navier-Stokes equations are well known. One may then expect that the small solution of the nonlinear equations (1.1) have the same decay rate as the linear one. Our work is devoted to proving the sharp time decay rate (for both upper and lower bound) for the nonlinear system.

In the case of one space dimension, Zeng [24] and Liu-Zeng [15] offered a detailed analysis of the solution to a class of hyperbolic-parabolic system through point-wise estimate, including the isentropic Navier-Stokes system. For multi-dimensional Navier-Stokes equations (and/or Navier-Stokes-Fourier system), the $H^s$ global existence and time-decay rate of strong solutions with the initial perturbation small in $H^s \cap L^1$ are obtained in whole space first by A. Matsumura and T. Nishida [17], [18]. When the small initial perturbation belongs to $H^3$ only, using a weighted energy method, A. Matsumura [16] showed the time-decay rate $(1+t)^{-\frac34}$ of upper bound in $L^\infty$-norm. Since then, there are concrete development on the upper bound time-decay estimates: the optimal $L^p$ (with $2\leq p \leq \infty$) upper bound decay rate was proved by G. Ponce [19], combining the spectral analysis on linearized system and the energy method for small initial perturbation in $L^1$. For the isentropic Navier-Stokes equations with artificial viscosity, D. Hoff and K. Zumbrun [6], [7] studied the Green's function and derived the $L^p$ ($1 \leq p\leq\infty$) upper bound time decay rate of diffusive waves for the small initial perturbation belongs to $H^m \cap L^1$ with $m\geq4$. Liu and Wang [14] studied the point-wise estimates of the Green function of the linearized isentropic Navier-Stokes system in 3D and then analyzed the coupling of nonlinear diffusion waves, obtained the optimal (upper bound) decay rate. These results were further extended to the exterior problem [12], [11], or the half space problem [9], [10], [8]. Recently, Guo and Wang in [5] developed a new general energy method for proving the optimal (upper bound) time decay rates of the solutions to the dissipative equations in the whole space, using a family of scaled energy estimates with minimum derivative counts and interpolations among them without linear decay analysis.

When additional external force is taken into account, the external force does affect the long time behavior of solutions. The upper bound of time decay rates were studied intensively, see for instance [1] and [2] on unbounded domain, [22], [23] on the convergence of the non-stationary flow to the corresponding steady flow when the initial date are small in $H^3 \cap L^{\frac65}$, and [4], [3], on the optimal $L^p-L^q$ upper bound decay rates for potential forces.

The main goal of current paper is to establish the sharp decay rate, on both upper and lower bounds, to the solutions of (1.1) using relatively simple energy method. We remark that similar results had been pursued by M. Schonbek [20], [21] for incompressible Navier-Stokes equations, and by Li, Matsumura-Zhang [13] for isentropic Navier-Stokes-Poisson system. Although they share the same spirit in obtaining the lower bound decay rates, the feature of the spectrum near zero exhibits quite different behaviors, leading to different analysis. For instance, we explored the elegant structure of the higher order nonlinear terms of Navier-Stokes, when choosing conservative variables: density and momentum. The conservative form of the sharp equations provided a natural derivative structure in these terms, leading to the possibility of a faster decay rate estimate. We will make a more detailed comparison later in this paper.

Define $n = \rho- \bar \rho$, and let $m = \rho u = (n+ \bar \rho)u$ be the momentum. We rewrite (1.1) as

where $\bar\mu = \frac{\mu}{\bar\rho}$, $\bar\nu = \frac{\nu}{\bar\rho}$, $c = \sqrt{p'(\bar \rho)}>0$ is the sound speed, and

It is this structure of $F$ that plays an important role in our analysis.

Our aim is to obtain a clear picture of the large time behavior of $U = (n, m)$ in $L^2({\mathop{\mathbb R\kern 0pt}\nolimits}^3)$ when $U_0 = (\rho_0-\bar \rho,\rho_0 u_0)$ is sufficiently smooth and small. We introduce the following initial value problem of the linearized Navier-Stokes system corresponding to (1.2):

where $\bar\mu = \frac{\mu}{\bar\rho}$, $\bar\nu = \frac{\nu}{\bar\rho}$, $c = \sqrt{p'(\bar \rho)}$. It is known that the $L^2$-norm of $\widetilde U = (\widetilde{n} , \widetilde{m} )$ decays at the optimal upper bound rate $(1+t)^{-\frac34}$ for generic small initial data, see for instance [18]. A detailed proof on the optimal lower and upper bound rate will be given in the section 3 of this paper. In section 4, we prove that $\|(U-\widetilde U)(\cdot, t)\|_{L^2}$ decays at a faster rate than $\|\widetilde U(\cdot, t)\|_{L^2}$, under some reasonable conditions on the initial data. Therefore, $\|U(\cdot, t)\|_{L^2}$ shares the sharp decay rate of $(1+t)^{-\frac34}$.

Notation. For $a \lesssim b$, we mean that there is a uniform constant $C$, which may be different on different lines, such that $a \leq Cb$. And $a \approx b$ stands for $a \lesssim b$ and $b\lesssim a$.

We now state our main result.

Theorem 1.1. Assume that $(n_0, m_0)\in L^1({\mathop{\mathbb R\kern 0pt}\nolimits}^3)\cap H^3({\mathop{\mathbb R\kern 0pt}\nolimits}^3)$, $\delta_0 = : \|(n_0,m_0)\|_{L^1({\mathop{\mathbb R\kern 0pt}\nolimits}^3)\cap H^3({\mathop{\mathbb R\kern 0pt}\nolimits}^3)}$ is sufficiently small, and

then there is a unique global classical solution $\widetilde U = (\widetilde{n}, \widetilde{m})\in \mathcal C([0,\infty); H^3({\mathop{\mathbb R\kern 0pt}\nolimits}^3))$ of the linearized system (1.3) satisfying for some positive constant $C$

and the initial value problem (1.2) has a unique solution $U = (n, m)\in \mathcal C([0,\infty); H^3({\mathop{\mathbb R\kern 0pt}\nolimits}^3))$. Moreover, let $n_h = n-\widetilde{n}$ and $m_h = m-\widetilde{m}$, then it holds that

As a consequence, there exists a positive constant $C_1$ such that

Remark 1.1. We remark that this theorem is valid under the condition (1.4) which is important in the lower bound estimate to the linearized problem. When (1.4) fails, the decay rate of the linearized system (1.3) depends on the order of the degeneracy of moments. Assume $(n_0, m_0)\in L^1\cap H^3$ and belong to certain appropriate weighted $L^p$ spaces, similar situation happened also in the incompressible Navier-Stokes equations, c.f. [20], [21]. We also note that our condition (1.4) is weaker than those in most of previous results where the differentiability of Fourier transform of initial disturbance is required in general.

Remark 1.2. In [13], Li, Matsumura-Zhang proved the lower bound decay rate of the linearized isentropic Navier-Stokes-Poisson system, they only require $|\widehat n_0(\xi)|>c_0>0$ for $|\xi|\ll 1$ with $c_0$ a constant due to the special structure of the spectrum from the help of the Poisson term. This condition is proposed in Fourier space, similar to (1.4) in some sense. In our case, the spectrum is different and the different structure leads to different sharp decay rates.

2.   Basic energy estimates

In what follows, we will set $n = \rho-\bar \rho$, $u = u-0$. We rewrite (1.1) in the perturbation form as

where $\bar \mu = \frac{\mu}{ \bar \rho }$, $\bar \nu = \frac{\nu}{ \bar \rho }$, $\gamma = \frac{p'(\bar \rho)}{\bar \rho^2}$, and the nonlinear functions $f$ and $g$ are defined by

We assume that there exist a time of existence $T>0$ and sufficiently small $\delta>0$, such that a priori estimate

holds for any $t\in[0,T]$. First of all, by (2.3) and Sobolev's inequality, we obtain that

Hence, we immediately have

where $f(n)$ and $g(n)$ are nonlinear functions of $n$ defined by (2.2).

Next, we begin with the energy estimates including $n$ and $u$ themselves. The following results is essentially due to A. Matsumura and T. Nishida [17], [18].

Theorem 2.1. Assume that $(n_0, u_0)\in H^3({\mathop{\mathbb R\kern 0pt}\nolimits}^3)$, then there exists a constant $\delta_0>0$ such that if

then the problem (2.1) admits a unique global solution $(n(t), u(t))$ satisfying that for all $t\geq0$,

where $C$ is a positive constant independent of time.

The proof of this theorem is divided into several subsections.

2.1.   Energy estimate for $0\leq k \leq 3$

For $k = 0$, multiplying the first equation in (2.1) by $\gamma n$ and the second equation in (2.1) by $u$, summing up and then integrating the result over ${\mathop{\mathbb R\kern 0pt}\nolimits}^3$ by parts. By virtue of Hölder's inequality, Sobolev's inequality and the fact (2.4), we obtain that

Now for $1\leq k \leq 3$, applying ${\nabla}^k$ to (2.1) and then multiplying the first equation by $\gamma{\nabla}^k n$ and the second equation by ${\nabla}^k u$, summing up and integrating over ${\mathop{\mathbb R\kern 0pt}\nolimits}^3$. For $k = 1$ we have

For $k = 2$ we have

For $k = 3$ we have

Summing up the above estimates, noting that $\delta>0$ is small, we obtain that

2.2.   Recover the dissipation estimates for $n$

For $0\leq k \leq 2$, applying ${\nabla} ^k$ to the second equation in (2.1) and then multiplying by ${\nabla}^{k+1} n$. The key idea is to integrate by parts in the $t$-variable and to use the continuity equation. Thus integrating the results by parts for both the $t$- and $x$-variables, we obtain for $k = 0$ that

for $k = 1$, we get

and for $k = 2$ we have

Plugging the above estimates, using the smallness of $\delta>0$, we obtain that

Proof of Theorem 2.1. Multiplying (2.13) by $\frac{2C_2\delta}{C_3}$, adding it with (2.9), with the help of smallness of $\delta>0$, we deduce that there exists a constant $C_5>0$ such that

Next, we define $\mathcal E(t)$ to be $C_5^{-1}$ times the expression under the time derivative in (2.14). Then we may write (2.14) as

Observe that since $\delta$ is small, then there exists a constant $C_6>0$ such that

Then integrating (2.15) directly in time, we get

Using a standard continuity argument along with classical local wellposedness theory, this closes the a priori assumption (2.3) if we assume $\|n_0\|_{H^3}+\|u_0\|_{H^3}\leq\delta_0$ is sufficiently small. We can then extend the solution globally in time and complete the proof of Theorem 2.1.

3.   Spectral analysis of the semigroup

In this section, we consider the initial value problem for the linearized Navier-Stokes system

where $\bar\mu = \frac{\mu}{\bar\rho}$, $\bar\nu = \frac{\nu}{\bar\rho}$, $c = \sqrt{p'(\bar \rho)}$.

In terms of the semigroup theory for evolutionary equations, the solution $(\widetilde{n}, \widetilde{m})$ of the linearized Navier-Stokes problem (3.1) can be expressed for $\widetilde U = (\widetilde{n}, \widetilde{m})^ t$ as

which gives rise to

where $B$ is defined as

What left is to analyze the differential operator $B$ in terms of its Fourier expression $A(\xi)$ and show the long time properties of the semigroup $S(t)$. Applying the Fourier transform to system (3.1), we have

where $\xi = (\xi_1,\xi_2,\xi_3)^t$, and $A(\xi)$ is defined as

The eigenvalues of the matrix $A$ can be computed by

which implies

The semigroup $e^{tA}$ is expressed as

where the project operators $P_i$ can be computed as

By a direct computation, we can verify the exact expression for the Fourier transform $\widehat G(t,\xi)$ of Green's function $G(t,x) = e^{tB}$ as

Indeed, we can make the following decomposition for $(\widetilde n, \widetilde m) = G \ast \widetilde U_0$ as

where

We further decompose the Fourier transform $\widehat N$, $\widehat M$ into low frequency term and high frequency term below.

Define

where $(\cdot)_1 = \chi(\xi)(\cdot)$, $(\cdot)_2 = (1-\chi(\xi))(\cdot)$, and $\chi(\xi)$ is a smooth cut off function such that

Then we have the following decomposition for $(\widetilde n, \widetilde m) = G \ast \widetilde U_0$ as

To derive the long time decay rate of solution, we need to use accurate approximation to the Fourier transform $\widehat G(t,x)$ of Green's function for both lower frequency and high frequency. In terms of the definition of the eigenvalues, we are able to obtain that it holds for $|\xi|\leq\eta$ for some small positive constant $\eta$ that

and we have

where

For the high frequency $|\xi|\geq\eta$, we are also able to obtain that it holds for $|\xi|\geq\eta$ that

and we have

where

Here $R_0$, $\eta$ are some fixed positive constants.

4.   Time decay rate for linear semigroup

In this section, we apply the spectral analysis to the semigroup for the linearized Navier-Stokes system. We will establish the $L^2$ and $L^p$ ($2\leq p \leq \infty$) time decay rate of the global solutions for the linearized Navier-Stokes system.

4.1.   $L^2$-time decay rate

With the help of the formula for Green's function in Fourier space and the asymptotic analysis on its elements, we are able to establish the $L^2$ time decay rate. Indeed, we have the $L^2$-time decay rate of the global strong solution to the problem for the linearized Navier-Stokes system as follows.

Proposition 4.1. Let $U_0 = (n_0, m_0)\in L^1({\mathop{\mathbb R\kern 0pt}\nolimits}^3)\cap H^l({\mathop{\mathbb R\kern 0pt}\nolimits}^3)$ with $l\geq3$, then $(\widetilde n,\widetilde m)$ solves the linearized Navier-Stokes system (3.1) and satisfies for $0\leq k\leq l$ that

where $C$ is a positive constant independent of time.

Proof. A straightforward computation together with the formula of the Green's function $\widehat G(t,\xi)$ gives

here and below, $R_0$, $\eta$ are some fixed positive constants. Therefore, we have the $L^2$-decay rate for $(\widetilde n, \widetilde m)$ as

And the $L^2$-decay rate on the derivatives of $(\widetilde n,\widetilde m)$ as

The proof of the Proposition 4.1 is completed.

It should be noted that the $L^2$-time decay rates derived above are optimal.

Proposition 4.2. Let $U_0 = ( n_0, m_0)\in L^1({\mathop{\mathbb R\kern 0pt}\nolimits}^3)\cap H^l({\mathop{\mathbb R\kern 0pt}\nolimits}^3)$ with $l\geq3$, assume that $M_n = \int_{{\mathop{\mathbb R\kern 0pt}\nolimits}^3}n_0(x) d x$ and $M_m = \int_{{\mathop{\mathbb R\kern 0pt}\nolimits}^3} m_0(x) dx$ satisfies that $M_n$, $M_m$ are at least not all zeros, then the solution $(\widetilde n,\widetilde m)$ of the linearized Navier-Stokes system (3.1) given by Proposition 4.1 satisfies for $0\leq k\leq l$

where $C$ is a positive constant independent of time.

Proof. We only show the case of $k = 0$ for simplicity, the argument applies to the other orders of derivatives. From the formula of the Green's function $\widehat G(t,\xi)$, we deduce that

here and below, $\eta$ is a sufficiently small but fixed constant.

It is easy to check that

We then calculate that

Since $n_0(x) \in L^1$ implies $\widehat{n}_0(\xi) \in C({{\mathop{\mathbb R\kern 0pt}\nolimits}^3})$. If $\widehat{n}_0(0) = \int_{{\mathop{\mathbb R\kern 0pt}\nolimits}^3}n_0(x) d x\neq 0$, we deduce that $\widehat{n}_0(\xi)\neq 0$ for $|\xi|\leq\eta$ when $\eta$ is sufficiently small. One finds that, when $M_n\neq 0$,

For $\widehat{m}_0$, a similar argument yields that, when $M_m\neq 0$, we have

When $M_n\neq 0$, $M_m\neq 0$, with the help of the above analysis, using $b\sim c|\xi|+O(|\xi|^3)$ for $|\xi|\leq \eta$, we obtain that

If $M_n\neq 0$, $M_m = 0$, and by the conituinity of $\widehat{m}_0$ near $\xi = 0$, there exists a small enough constant $\epsilon$ such that $\epsilon\to0$ as $\xi\to 0$, and

We thus use the help of spherical coordinates and the change of variables $r = |\xi|\sqrt{t}$ to obtain that

In the case of $M_n = 0$, $M_m\neq0$, we can use a similar argument to obtain that

Combining the above estimates (4.1), (4.2), (4.3), (4.4) and (4.5), we obtain the lower bound of the time decay rate for ${\widetilde n}(t,x)$ as

The lower bound of the time decay rate for ${\widetilde m}(t,x)$ can be shown in a similar fashion. It is not difficult to derive that

then we find that

We then calculate that

A direct computation gives rise to

Combining the above estimates (4.6), (4.7) and (4.8), we obtain the lower bound of the time decay rate for ${\widetilde m}(t,x)$ as

Then the proof of Proposition 4.2 is completed.

4.2.   $L^p$-time decay rate

In this subsection, we establish the following $L^p$-time decay rate of the global strong solution to the linearized Navier-Stokes system with $p \in [2,+\infty]$.

Proposition 4.3. Let $U_0 = (n_0,m_0)\in L^1({\mathop{\mathbb R\kern 0pt}\nolimits}^3)\cap W^{l,p}({\mathop{\mathbb R\kern 0pt}\nolimits}^3)$ with $l\geq 3$, then $(\widetilde n,\widetilde m)$ solves the linearized Navier-Stokes system (3.1) and satisfies for $0\leq k\leq l$ and $p \in [2,+\infty]$ that

where $C$ is a positive constant independent of time.

To prove Proposition 4.3, the following two lemmas in [6] are helpful.

Lemma 4.1. Let $n\geq 1$ and assume that $\hat f(\xi) \in L^\infty \cap C^{n+1}({\mathop{\mathbb R\kern 0pt}\nolimits}^n/\{0\})$, with

where $\sigma_1, \sigma_2>0$ and $n>2-2\sigma_2$. Then $\hat f(\xi)$ is continuous at $0$ and $\infty$, and

where $m_1\in L^1({\mathop{\mathbb R\kern 0pt}\nolimits}^n)$ satisfies $\|m_1\|_{L^1({\mathop{\mathbb R\kern 0pt}\nolimits}^n)} \leq C(C')$, $m_2$ is the constant

and $\delta$ is the Dirac distribution. In particular, $\hat f(\xi)$ is a strong $L^p$ multiplier, $1\leq p \leq \infty$, in the sense that, for any $g\in L^p$,

where $C$ depends only on $|m_2|\leq \| \hat f\|_{L^\infty}$ and the constant $C'$ above.

Lemma 4.2. Let $\hat g(t,\xi) = \hat K(t,\xi)\hat f(\xi)$, where $\hat K(t,\xi) = e^{-\vartheta|\xi|^2 t}$, $\hat f(\xi)\in L^\infty\cap C^{n+1}({\mathop{\mathbb R\kern 0pt}\nolimits}^n)$, and

Then ${\nabla}_x ^\alpha g(t,\cdot)\in L^p$ for $t>0$, and for all $\alpha$, $1\leq p \leq \infty$, we have

In particular, $\widehat{{\nabla}_x ^\alpha g(t,x)} = (i\xi)^\alpha \hat g(t,\xi)$ is a strong $L^p$ multiplier, with norm bounded by $C(|\alpha|,\vartheta)C't^{-\frac{|\alpha|}2}$, where the constant $C(|\alpha|,\vartheta)$ depends only on $|\alpha|$ and $\vartheta$.

Now let us turn to the proof of Proposition 4.3.

Proof of Proposition 4.3. We first analyze above higher frequency terms denoted by $\widehat {(\cdot)}_2$. Recall that

We shall prove that the higher frequency terms are $L^p$ Fourier multipliers with an exponential time decay coefficient $C e^{-c_1t}$ for some constants $c_1>0$. For simplicity, we only show that $\widehat {\mathcal N}_2$ is an $L^p$ Fourier multiplier at higher frequency as follows. It holds

By a direct computation, it is easy to verify

which gives rise to

here and below, $R>0$ is a given constant. Thus, from Lemma 4.1 it follows that the inverse Fourier transform of the term $(1-\chi(\cdot))\left(e^{\lambda_2 t}+\frac{\lambda_2 e^{\lambda_2 t}}{\lambda_1-\lambda_2}\right)$ is an $L^p$ multiplier with the coefficient $Ce^{-c_1t}$. The other part of $\widehat {\mathcal N}_2$ at higher frequency can be written as

We can regard $e^{-\frac12 (2\bar\mu+\bar\nu) |\xi|^2 t}$ as the function $K(t,\xi)$ of Lemma 4.2, and the rest term satisfies the condition. Thus, the inverse Fourier transform of $(1-\chi(\cdot))\frac{\lambda_2 e^{\lambda_1 t}}{\lambda_1-\lambda_2}$ is also an $L^p$ multiplier with the coefficient $Ce^{-c_1t}$. These facts imply that $\widehat {\mathcal N}_2$ at higher frequency is an $L^p$ multiplier with the coefficient $Ce^{-c_1t}$. Applying the similar analysis to the terms $\widehat {\mathfrak N}_2$, $\widehat {\mathcal M}_2$, and $\widehat {\mathfrak M}_2$, we can show that their inverse Fourier transform are all $L^p$ multiplier with the constant coefficient $Ce^{-c_1t}$. Then

for all integer $k\geq 0$, and $p\in[2,\infty]$.

We also need to deal with the corresponding lower frequency terms denoted by $\widehat {(\cdot)}_1$. Recall that

which imply that for $|\xi|\leq\eta$ that

for some constants $c_2>0$. Thus, by Hausdroff-Young's inequality with $p\in[2, +\infty]$, we can obtain

Combining (4.9) and (4.10), we finally have for $t>0$ that

The proof of Proposition 4.3 is completed.

5.   $L^2$-time decay rate for nonlinear system

We are ready to prove Theorem 1.1 on the sharp time decay rate of the global solution to the initial value problem for the nonlinear Navier-Stokes system.

In what follows, we will set $n_h = n-\widetilde n$ and $m_h = m-\widetilde m$, then we have

where $\bar\mu = \frac{\mu}{\bar\rho}$, $\bar\nu = \frac{\nu}{\bar\rho}$, $c = \sqrt{p'(\bar \rho)}$, and

Denote $U_h = (n_h, m_h)^t$, we have the equivalent form of system (5.1) in vector form

where the nonlinear term $H(\widetilde U, U_h) = (0, F(\widetilde U, U_h))^t$. Thus, we can represent the solution in term of the semigroup

which $(n_h, m_h)$ can be decomposed as

Furthermore, in view of the above definition for $\widehat{\mathfrak N}(\xi)$ and $\widehat{\mathfrak M}(\xi)$, it is easy to verify for some constants $c_3>0$, $c_4>0$, $R_0>0$, we discover that

Thus, applying a similar argument as in the proof of Proposition 4.1, we have

for any non-negative integer $k$ and

For readers' convenience, we show how to estimate $\|{\nabla}^k {\mathfrak M}\ast H(t)\|_{L^2}$ as an example. The other two estimates can be obtained by the similar argument. Indeed,

5.1.   $L^2$-time decay rate

In this subsection, we establish the faster decay rate for $(n_h, m_h)$. We will start with an a priori assumption on a carefully chosen quantity $\Lambda(t)$ defined in (5.8), and then later prove a better estimate with the help of the smallness of initial data.

We begin with following Lemma.

Lemma 5.1. Let $r_1, r_2>0$ be real, one has

and

where $\epsilon>0$ is a small but fixed constant.

Proposition 5.1. Under the assumptions of Theorem 1.1, the solution $(n_h, m_h)$ of the nonlinear system (5.1) satisfies for $k = 0,1,2$ that

where $C$ is a positive constant independent of time.

From (5.7), we deduce

which implies for a smooth solution $(n,m)$ satisfying $\|(n,m)\|_{H^3}<\infty$ that

Define

Proposition 5.2. Under the assumptions of Theorem 1.1, if for some $T>0$, $\Lambda(t) \leq \delta_0^{\frac12}$ for any $t\in[0,T]$, then it holds that

where $C$ is a positive constant independent of time.

The proof of this Proposition 5.2 consists of following three steps.

5.2.   Step 1: The basic energy estimates

Starting with (5.4), (5.5), (5.6) and (5.8), we have after a complicate but straightforward computation that

It is easy to verify that

Indeed, by virtue of Hölder's inequality and Gagliardo-Nirenberg's inequality, we obtain that

which implies that

Furthermore, exactly as in the estimate of the high order derivatives, we have

Similarly, it holds that

Thus, we also get that

Finally, we have

5.3.   Step 2: The higher order energy estimates

In this subsection, we will close the a priori estimates and complete the proof of Proposition 5.2. For this purpose, we need to derive the time decay rate of higher order derivatives of $(n_h,m_h)$. We will establish the following lemma.

Lemma 5.2. Under the assumption of Theorem 1.1, one has

In particular, it holds that

Proof. First of all, in view of (2.12), recovering the dissipation estimate for $n$, we see that

Summing up (2.7) and (2.8) in the energy estimate for $(n,u)$, we can directly derive

Multiplying (5.12) by $\epsilon_1\frac{C_3}{C_2}$ with $\epsilon_1>0$ a small but fixed constant, adding it with (5.13), we deduce that there exists a constant $C_4>0$ such that

Next, we define

Observe that since $\epsilon_1\frac{C_3}{C_2}$ is small, then there exists a constant $C_5>0$ such that

Then we arrive at

Denote $S(t) = \Big\{\xi\big| |\xi| \leq \sqrt{\frac{3(1+\gamma)}{C_4}}(1+t)^{-\frac12}\Big\}$ the time-dependent $n$-dimensional sphere. This decomposition allows us to estimate $L^2$ time decay depend on $(\widehat {n}, \widehat {u})$ for frequency values $\xi \in S(t)$, then we obtain that

Hence we have

Multiplying the above equation by $(1+t)^5$, we obtain that

Integrating it with respect to time from $0$ to $T$, then we have

which implies that

Finally, we have

This completes the proof of this Lemma.

5.4.   Step 3: Close the estimates

In this subsection, we first combine the above a priori estimates of (5.8), (5.9), (5.10), (5.11) and Lemma 5.2 together to give the proof of the Proposition 5.2. In deed, for any $t\in[0,T]$, we have shown that

With the help of standard continuity argument, Proposition 5.2 and the smallness of $\delta_0>0$, implies that $\Lambda(t)\leq C\delta_0^{\frac34}$ for any $t>0$. Moreover, we deduce the time decay estimate for $(n_h, m_h)$ from (5.9), (5.10), (5.11), Lemma 5.2 and (5.14) that

Consequently, for any $t\in[0,T]$ we have

From (5.11) and (5.15), thus we also get that

For ${\nabla}^3 m_h$, in view of the (5.6), we see that

Hence, we finish the proof of the Proposition 5.1. Theorem 1.1 follows.

Acknowledgments

Y. Chen is partially supported by the China Postdoctoral Science Foundation under grant 2019M663198, Guangdong Basic and Applied Basic Research Foundation under grant 2019A1515110733, NNSF of China under grants 11801586, 11971496 and China Scholarship Council. The research of R. Pan is partially supported by National Science Foundation under grants DMS-1516415 and DMS-1813603, and by National Natural Science Foundation of China under grant 11628103. L. Tong's research is partially supported by China Scholarship Council.