# Quasi-periodic solutions for a nonlinear non-autonomous Hamiltonian system

Quasi-periodic solutions for a nonlinear non-autonomous Hamiltonian system

Yi WangHui Wang Min Zhang Jie Rui

School of Mathematics and Quantitative Economics, Shandong University of Finance and Economics, Jinan 250014, China

College of Science, China University of Petroleum, Qingdao 266580, China

Corresponding Author Email:
yiwang8080@126.com
Page:
259-271
|
DOI:
https://doi.org/10.3166/JESA.51.259-271
|
Accepted:
|
Published:
31 December 2018
| Citation

OPEN ACCESS

Abstract:

The quasi-periodic solutions of nonlinear Hamiltonian system are important tools to enhance our understanding of dynamic behaviours. Therefore, this paper probes into a popular, completely resonant nonlinear beam equation. In the equation model, there is a nonlinear term periodic in the space variable and quasi-periodic in the time variable. The external frequency vector is 2-dimensional. Using the Kolmogorov-Arnold-Moser (KAM) method and the normal form, the author proved the existence of quasi-periodic solutions with two frequencies and gave the analytical expression. The solutions are small amplitude and linearly stable. The research findings shed new light on measurement estimation and normal form technique, provide new insights into the dynamics of beam equation, and promote the application of the KAM method.

Keywords:

kolmogorov-arnold-moser (KAM) method, hamiltonian, beam equation, quasi-periodic solution, normal form

1. Introduction

This paper discusses the existence of quasi-periodic solutions for a beam equation

$u_{t t}+u_{x x x x}+f(\omega t, x, u)=0, x \in[0, \pi]$          (1.1)

under the hinged boundary conditions

$u(t, 0)=u_{x x}(t, 0)=u(t, \pi)=u_{x x}(t, \pi)=0$         (1.2)

where $\omega=\left(\omega_{1}, \omega_{2}\right) \in[\eta, 2 \eta]^{2}$ is a frequency vector with $\eta>0 ; f(\omega t, x, u)$ is a quasi-periodic nonlinear term in the time variable, and $f(\omega t, x, u)=f(\vartheta, x, u)(\vartheta \in$ $\left.\mathbb{T}^{2} :=\mathbb{R}^{2} / 2 \pi \mathbb{Z}^{2}\right)$ is a real analytic function in $\vartheta$ and $x .$

The purpose of the discussion is to verify whether the small amplitude quasi-periodic solutions of $u_{t t}+u_{x x x x}=0$ can persist under perturbation, whether the finite-dimensional tori is linearly stable, and whether quasi-periodic solutions have zero Lyapunov exponents.

For non-autonomous Hamiltonian systems like Equation (1.1), their quasi-periodic solutions are mainly investigated by the Lyapunov-Schmidt decomposition. However, the quasi-periodic solutions thus obtained tend to be global, failing to provide dynamical information around equilibrium points. Here, the Kolmogorov-Arnold-Moser (KAM) method is adopted to solve the problem.

The KAM theory, named after its proposer Kolmogorov, Arnold, and Moser, is one of the most important mathematical achievements in the 20th century. Later, Wayne, Kuksin, and Pöschel developed the infinite-dimensional KAM theory, which produces quasi-periodic solutions with dynamic properties like linear stability (Chen, 2017; Chen et al., 2017; Cao and Yuan, 2017; Si and Si, 2017; Si and Si, 2018) and vanishing Lyapunov exponents.

The KAM method can be applied to examine the Hamiltonian partial differential equations (PDEs) in the following manner: transforming nonlinear equations into infinite-dimensional Hamiltonian systems; constructing canonical transformations that can change the Hamiltonians to suitable Birkhoff normal forms; looking for quasi-periodic solutions though KAM iterations, that is, setting up a KAM theorem.

Much research has been done on the quasi-periodic solutions of nonlinear beam equations (Eliasson et al., 2016; Geng and You, 2003; Geng and You, 2006; Geng and Zhou, 2018; Liang and Geng, 2006; Procesi, 2010). However, there is only a few reports on those of complete resonant equations. Geng and You (2006) tackle a complete resonant beam equation with a nonlinear term $u^{3}$

. Tuo and Si (2015) probe into a beam equation with nonlinearity $\phi(t) u^{5}$  (Gao and Liu, 2017; Ge and Geng, 2018).

In this paper, it is assumed that $f$ in Equation $(1.1)$ has a special nonlinear form $f(t, x, u)=\delta \psi(\omega t, x) u^{3},$ where $\delta$ is a small positive parameter and $\psi$ is quasi- periodic in $t$ and periodic in $x$ . This model is very difficult to solve because of the dependence of nonlinearity on time and space variables, but it is widely applicable.

Equation $(1.1)$ is a perturbation of the linear beam equation $u_{t t}+u_{x x x x}=0$ whose solution can be written as $u(t, x)=\sum_{j \in J} q_{j}(t) \phi_{j}(x), q_{j}(t)=I_{j} \cos \left(j^{2} t+\right.$ $\left.\varphi_{j}^{0}\right) .$ Here, for $j \in Z^{+}, \phi_{j}(x)=\sqrt{\frac{2}{\pi}} \sin j x ; \quad J$ is any subset of $Z^{+} :=\{1,2, \cdots\}$

;amplitudes $I_{j} \geq 0$ and $\varphi_{j}^{0}$ are initial phases. The solutions travel on a rotational torus, which is finite- or infinite-dimensional. Every torus is linearly stable. The Lyapunov exponents of all solutions are zero. Unfortunately, not all the invariant manifolds will be preserved under the perturbation of $f,$ owing to the numerous resonances and the strong perturbation of $f$ on solutions of large amplitude.

This paper innovatively transforms the Hamiltonian into its Birkhoff normal form, despite falling short of the zero-momentum conditions. The perturbation was divided into two parts to overcome the difficulty of small divisor. One part satisfies zero-momentum conditions while the other part does not. Thus, several conditions were added in Section 3. Then, it is necessary to estimate the measure of the parameter $\omega$

, so as to maximize the number of parameters satisfying these conditions. Fortunately, the growth of eigenvalues is quartic, which is crucial for measure estimation. The KAM iterations here are in the standard form (Liu and Yuan, 2014), and are thus omitted.

The remainder of this paper is organized as follows: Section 2 transforms the equation into an infinite-dimensional Hamiltonian system; Section 3 obtains the Birkhoff normal form; Section 4 relies on the normal form to prove the existence of quasi-periodic solution and give an analytic expression.

2. Hamiltonian setting

Firstly, Equation $(1.1)$ was converted to a Hamiltonian system. Under Equation $(1.2),$ the operator $B=\frac{d^{4}}{d x^{4}}$ has eigenvalues $\zeta_{j}=j^{4}$ and eigenfunctions $\phi_{j}(x)=$ $\sqrt{\frac{2}{\pi}} \sin j x,$ where $j \in \mathbb{Z}^{+} :=\{1,2, \cdots\} .$ Let $D_{1}\left(\sigma_{1}\right) :=\left\{\vartheta| | \operatorname{Im} \vartheta |<\sigma_{1}\right\},|\psi|_{2 a} :=$ $\sup _{x \in D_{2}(2 a)}|\psi(\vartheta, x)|$ for $\vartheta \in D_{1}\left(\sigma_{1}\right) :=\{x| | \operatorname{Im} x |<2 a\},$ and $|\psi|_{\sigma_{1}, 2 a} :=\sup _{(\vartheta, x) \in D_{1}\left(\sigma_{1}\right) \times D_{2}(2 a)}|\psi(\vartheta, x)|$.

It is assumed that $<\cdot,>$ is the standard inner product in $\mathbb{C}^{2} ;(\cdot, \cdot)$ is the scalar product in $L^{2}[0, \pi]$ , the space of real-valued sequences is $l^{a, s}=l^{a, s}(\mathbb{R}) :=\left\{q=\left(q_{1}, q_{2}, \cdots\right),\left(\|q\|_{a, s}\right)^{2}=\sum_{i \geq 1}\left|q_{i}\right|^{2} i^{2 s} e^{2 a i}<\infty\right\}$ $\left(a>0, s>\frac{1}{2}\right)$.

$\sigma_{1}>0$ and $\sigma_{1}$ has a positive lower bound $\tilde{\sigma}_{1}, a$ is a positive real number, and " measure ", refers to the Lebesgue measure. For function $\psi,$ the following assumptions were put forward:

(Al) $\psi$ has a Fourier expansion $\psi(\vartheta, x)=\psi_{0}+\sum_{k \in Z^{2} \backslash\{0\}} \psi_{k}(x) e^{i<k, \vartheta>}$ with $0 \neq$ $\psi_{0} \in \mathbb{R} .$

(A2) $\psi$ can analytically extend to $D_{1}\left(\sigma_{1}\right) \times D_{2}(2 a)$ with $|\psi|_{\sigma_{1}, 2 a}<\infty$.

$(\mathrm{A} 3) \partial_{x}^{2 k+1} \psi(\vartheta, 0)=0, \forall k \in \mathbb{N}$.

By introducing $\partial_{t} u=v, \partial_{t} v+B u=-\delta \psi(\omega t, x) u^{3},$ Equation $(1.1)$ can be changed to a Hamiltonian system $H=\frac{1}{2}(v, v)+\frac{1}{2}(B u, u)+\frac{\delta}{4} \int_{0}^{\pi} \psi(\omega t, x) u^{4} d x .$

If $u(t, x)=\sum_{j \geq 1} \frac{q_{j}(t)}{4 \sqrt{\zeta_{j}}} \phi_{j}(x), v(t, x)=\sum_{j \geq 1} \sqrt{\zeta_{j}} p_{j}(t) \phi_{j}(x)$,

Where $q=\left(q_{1}, q_{2}, \cdots\right), p=\left(p_{1}, p_{2}, \cdots\right)$ and $p, q \in l^{a, s} .,$ then the Hamiltonian can be transformed to $H=\Lambda+\delta G,$ and

$\Lambda=\frac{1}{2} \sum_{j \geq 1} \sqrt{\zeta_{j}}\left(q_{j}^{2}+p_{j}^{2}\right), G=\frac{1}{4} \int_{0}^{\pi} \psi(\omega t, x)\left(\sum_{j \geq 1} \frac{q_{j}(t)}{4} \phi_{j}(x)\right)^{4} d x$.

Then, the Hamiltonian system can be expressed as:

$\dot{q}_{j}=\frac{\partial H}{\partial p_{j}}=\sqrt{\zeta_{j}} p_{j}, \dot{p}_{j}=-\frac{\partial H}{\partial q_{j}}=-\sqrt{\zeta_{j}} q_{j}-\delta \frac{\partial G}{\partial q_{j}}, j \geq 1$        (2.1)

The corresponding symplectic structure is $\sum d q_{i} \wedge d p_{i}$ on $l^{a, s} \times l^{a, s} .$ According to Geng and You (2003), if the solution of Equation (2.1)$(p(t), q(t))$ is real analytic for $t \in I,$ then for $(t, x) \in \times[0, \pi],$

$u(t, x)=\sum_{j \geq 1} \frac{q_{j}(t)}{4 \sqrt{\zeta_{j}}} \phi_{j}(x)$         (2.2)

must be a real analytic classical solution of Equation (1.1), where $I$ is a real interval. Thus, this paper attempts to find a solution with the form (2.2).

Then, action-angle variables $J \in \mathbb{R}^{2}$ and $\vartheta \in \mathbb{T}^{2}$ were introduced to obtain an autonomous system. In this way, the Hamiltonian and the Hamiltonian system can be transformed into

$H=<\omega, J>+\frac{1}{2} \sum_{j \geq 1} \sqrt{\zeta_{j}}\left(q_{j}^{2}+p_{j}^{2}\right)+\delta G(q, \vartheta)$    (2.3)

and

$\dot{q}_{j}=\frac{\partial H}{\partial p_{j}}, \dot{p}_{j}=-\frac{\partial H}{\partial q_{j}}, \dot{\vartheta}=\omega, j=-\delta \frac{\partial G}{\partial \vartheta}=-\delta \frac{\partial \int_{0}^{\pi} \chi d x}{\partial \vartheta},(j \geq 1)$

The corresponding symplectic structure becomes $d \vartheta \wedge d J+\sum d q_{i} \wedge d p_{i} .$ The following lemma can be proved by the method for Lemma 2.3 in Wang et al. (2018) .

Lemma 2.1 The gradient $\frac{\partial G}{\partial q}$ is real analytic and satisfies $\left\|\frac{\partial G}{\partial q}\right\|_{a, s}=O\left(\left(\|q\|_{a, s}\right)^{3}\right)$.

3. Brikhoff normal form

This section transforms the Hamiltonian into a Birkhoff normal form. The complex coordinates $\mathbf{z}=\left(\mathbf{z}_{\mathbf{1}}, \mathbf{z}_{2}, \cdots\right), \quad \overline{\mathbf{z}}=\left(\overline{\mathbf{z}}_{\mathbf{1}}, \overline{\mathbf{z}}_{\mathbf{2}}, \cdots\right)$,  and $\mathbf{z}, \overline{\mathbf{z}} \in \boldsymbol{l}^{a, \boldsymbol{s}}(\mathbb{C})$ were adopted, where$Z_{i}=\frac{q_{i}+i p_{i}}{\sqrt{2}}, \overline{Z}_{i}=\frac{q_{i}-i p_{i}}{\sqrt{2}}$ for $i \in \mathbb{Z}^{+}$. Then, a real analytic Hamiltonian can be obtained as:

$H=\Lambda+\delta G$        (3.1)

where $\Lambda=<\omega, J>+\sum_{j} \sqrt{\zeta}_{j} z_{j} \overline{z}_{j}, \quad G=\frac{1}{4} \int_{0}^{\pi} \psi(\vartheta, x)\left(\sum_{j \geq 1} \frac{z_{j}+z_{j}}{\sqrt{4} z_{j}} \phi_{j}(x)\right)^{4} d x$

The corresponding symplectic structure becomes $d \vartheta \wedge d J+i \sum_{i} d z_{i} \wedge d \overline{z}_{i}$. Moreover, we have

\boldsymbol{G}=\frac{1}{16} \sum_{\iota_{1}, t_{2}, t_{3}, t_{3}, t_{4} \in \mathbb{Z}^{+}, t_{1} \pm t_{2} \pm t_{3} \pm t_{4}=0} \frac{\boldsymbol{G}_{t_{1} t_{2} t_{3} t_{4}}}{t_{1} \boldsymbol{t}_{2} \boldsymbol{l}_{3} \boldsymbol{l}_{4}}\left(\mathbf{z}_{t_{1}}+\overline{\mathbf{z}}_{t_{1}}\right)\left(\mathbf{z}_{t_{2}}+\overline{\mathbf{z}}_{t_{2}}\right)\left(\mathbf{z}_{t_{3}}+\overline{\mathbf{z}}_{t_{3}}\right)\left(\mathbf{z}_{t_{4}}+\overline{\mathbf{z}}_{t_{4}}\right)+\frac{1}{16} \sum_{|k| \geq 1, \iota_{1}, l_{2}, l_{3}, l_{4} \in \mathbb{Z}^{+}} \frac{G_{k, t_{1} i_{2} t_{3} t_{4}}}{\iota_{1} t_{2} t_{3} t_{4}} e^{i<k, \vartheta>}\left(z_{t_{1}}+\overline{z}_{t_{1}}\right)\left(z_{t_{2}}+\overline{z}_{t_{2}}\right)\left(z_{t_{3}}+\overline{z}_{t_{3}}\right)\left(z_{t_{4}}+\overline{z}_{t_{4}}\right), where G_{t_{1} t_{2} t_{3} t_{4}}=\psi_{0} \int_{0}^{\pi} \phi_{l_{1}} \phi_{l_{2}} \phi_{t_{3}} \phi_{l_{4}} d x (3.2) and G_{k, t_{1}, t_{2} t_{3} t_{4}}=\int_{0}^{\pi} \psi_{k}(x) \phi_{t_{1}} \phi_{t_{2}} \phi_{t_{3}} \phi_{t_{4}} d x,|k| \geq 1 (3.3) It is obvious that G_{\iota_{1} \iota_{2} l_{3} l_{4}}=0 . unless \iota_{1} \pm \iota_{2} \pm \iota_{3} \pm \iota_{4}=0 and G_{\iota_{1} l_{2} l_{1} l_{2}}=\frac{\psi_{0}}{2 \pi}\left(2+\delta_{l_{1} l_{2}}\right) (3.4) where \delta_{t_{1} t_{2}}=1 for \iota_{1}=\iota_{2}, and \delta_{t_{1} t_{2}}=0 for \iota_{1} \neq \iota_{2}. Next, an admissible set \mathscr{L} :=\left\{\left(n_{1}, n_{2}\right) | n_{1}, n_{2} \text { are odd, } n_{1} \neq 7 \bmod (14), n_{2}>\right. \left.6 n_{1}^{2}\right\} was selected, which satisfies the Definition 3.1 in Liang and Geng (2006) . Three sets of vectors \left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \mathbb{Z}_{+}^{4} . were defined for each index set \mathscr{E} : the set \Delta_{0} that l_{1}, l_{2}, l_{3}, and \iota_{4} are all in \mathscr{E}, the set \Delta_{j} that 4-j of \iota_{1}, l_{2}, l_{3}, and l_{4} are in \mathscr{E} for j=1,2,, and the set \Delta_{3} that none or only one of l_{1}, l_{2}, l_{3}, and l_{4} is in \mathscr{E} . Let \mathscr{B}_{0}= \left\{\left(l_{1}, l_{2}, l_{3}, l_{4}\right) \equiv\left(l_{1}, l_{2}, l_{1}, l_{2}\right)\right\}, \mathscr{E}_{1}=\mathscr{E}_{0} \cap \Delta_{0} and \mathscr{E}_{2}=\mathscr{E}_{0} \cap \Delta_{2} . The next step is to construct a Hamiltonian \mathrm{S} and use its vector-field X_{\mathcal{S}} to transform Equation (3.1) into a fourth-order partial Birkhoff form, so as to study it as a perturbation of a nonlinear integrable system. However, the divisors have to be assumed as nonzero because of the small divisors of the Hamiltonian. Thus, it is necessary to estimate the measure of parameters which make the divisors zero. For this purpose, notations \overline{\Delta} :=\Delta_{0} \cup \Delta_{1} \cup \Delta_{2} and \overline{\Delta} :=\left(\Delta_{0} \backslash \mathscr{E}_{1}\right) \cup \Delta_{1} \cup\left(\Delta_{2} \backslash \mathscr{E}_{2}\right) were introduced. Lemma 3.1 If \left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \overline{\Delta} and k are not zero and \delta is sufficiently small, then there is a set \overline{\Omega} \subset[\eta, 2 \eta]^{2} satisfying that, for each \omega \in \overline{\Omega} and \pm \sqrt{\zeta_{\iota_{1}}} \pm \sqrt{\zeta_{\iota_{2}}} \pm \sqrt{\zeta_{\iota_{3}}} \pm \sqrt{\zeta_{\iota_{3}}} \pm \sqrt{\zeta_{\iota_{3}}} \pm \sqrt{\zeta_{\iota_{4}}} \neq 0, | \pm \sqrt{\zeta_{t_{1}}} \pm \sqrt{\zeta_{t_{2}}} \pm \sqrt{\zeta_{t_{3}}} \pm \sqrt{\zeta_{t_{4}}}+<k, \omega>| \geq \frac{\eta_{\delta^{\frac{1}{3}}}}{|k|^{4}} (3.5) Moreover, meas \overline{\Omega} \geq \eta^{2}\left(1-C_{2} \delta^{\frac{1}{3}}\right), where C_{2} is a constant depending on \eta, n_{1}, and n_{2} . Proof Assuming that: h_{t_{1} t_{2} t_{3} t_{4}, k}=\pm \sqrt{\zeta_{t_{1}}} \pm \sqrt{\zeta_{t_{2}}} \pm \sqrt{\zeta_{t_{3}}} \pm \sqrt{\zeta_{t_{4}}}+<k, \omega> R_{l_{1} l_{2} l_{3} l_{4}, k}=\left\{\omega \in[\eta, 2 \eta]^{2} :\left|h_{l_{1} l_{2} l_{3} l_{4}, k}\right|<\frac{\eta \delta^{3}}{|k|^{4}}\right\} \Omega^{1}=\cup_{|k| \geq 1} \cup_{\left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{1}} R_{l_{1} l_{2} l_{3} l_{4}, k}, and \Omega^{2}=\cup_{|k| \geq 1} \cup_{\left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{2}} R_{l_{1} l_{2} l_{3} l_{4}, k} . It is evident that \tilde{\Omega}=\Omega^{0} \cup \Omega^{1} \cup \Omega^{2} . For hyperplanes \pm \sqrt{\zeta_{t_{1}}} \pm \sqrt{\zeta_{t_{2}}} \pm \sqrt{\zeta_{t_{3}}} \pm \sqrt{\zeta_{t_{4}}}+<k, \omega>=\pm \frac{\eta_{\delta}^{\frac{1}{3}}}{|k|^{4}}. We have \operatorname{Measure} R_{t_{1} \iota_{2} t_{3} t_{4}} \leq 2|k|^{-1} \sqrt{2} \eta \frac{2 \eta \delta^{\frac{1}{3}}}{|k|^{4}} \leq \frac{4 \sqrt{2} \delta^{\frac{1}{3}}}{|k|^{5}} \eta^{2}. Hence, Measure R_{t_{1} t_{2} t_{3} t_{4}} \leq C \frac{\eta^{2} \delta_{3}^{\frac{1}{3}}}{\left|k_{1}\right|^{5}}, where C is an absolute constant. Note that \#\left\{k \in Z^{2} :|k|=l\right\} \leq 2^{2} l, l \in Z^{+} (3.6) Case I. If \left(\iota_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{0}, then it can be deduced from (3.6) that: \Omega^{0} \leq C \sum_{|k| \geq 1} \frac{\eta^{2} \delta^{\frac{1}{3}}}{|k|^{5}}\left(n_{2}-n_{1}+1\right)^{4} \leq C\left(n_{2}-n_{1}+\right.1) ^{4} \eta^{2} \delta^{\frac{1}{3}} \sum_{1 \leq|k|=l} \frac{1}{l^{5}} 2^{2} l. since \sum_{l \geq 1} \frac{1}{l^{4}} is convergent, Measure \Omega^{0} \leq C \eta^{2} \delta^{\frac{1}{3}} , and C is dependent of n_{1}, n_{2} and \eta . Case II. For \left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{1}, it is assumed that l_{4} \notin \mathscr{L} . The other cases can be treated by analogy. Then, it can be derived that |<k, \omega>\pm \sqrt{\zeta_{l_{1}}} \pm \sqrt{\zeta_{l_{2}}} \pm \sqrt{\zeta_{l_{3}}}| \leq 2 \eta|k|+3 n_{2}^{2}. If \left|l_{4}\right|>\sqrt{2 \eta|k|+3 n_{2}^{2}+1} and \delta is sufficiently small, \begin{aligned}\left|h_{t_{1} t_{2} t_{3} t_{4}, k}\right| \geq &| \pm \sqrt{\zeta_{t_{4}}}|-|<k, \omega>\pm \sqrt{\zeta_{t_{1}}} \pm \sqrt{\zeta_{t_{2}}} \pm \sqrt{\zeta_{t_{3}}}|>2 \eta|k|+3 n_{2}^{2}+\\ 1-\left(2 \eta|k|+3 n_{2}^{2}\right) &=1>\frac{\eta^{2} \delta_{3}^{1}}{|k|^{4}} \cdot | \end{aligned} Thus, it only needs to discuss 1 \leq \iota_{4} \leq \sqrt{2 \eta|k|+3 n_{2}^{2}+1}. Therefore, Measure \Omega^{1} \leq C \sum_{|k| \geq 1} \frac{\eta^{2} \delta^{\frac{1}{3}}}{|k|^{4}|k|}\left(n_{2}-n_{1}+1\right)^{3} \sqrt{2 \eta|k|+3 n_{2}^{2}+1} \leq C \eta^{2} \delta^{\frac{1}{3}}\left(n_{2}-\right.\left.n_{1}+1\right)^{3} \sum_{|k| \geq 1} \frac{1}{|k|^{4}} \leq C \eta^{2} \delta^{\frac{1}{3}}\left(n_{2}-n_{1}+1\right)^{3} \sum_{l \geq 1} 2^{2} l \frac{1}{l^{4}} \leq C \eta^{2} \delta^{\frac{1}{3}} and C is dependent of n_{1}, n_{2} and \eta . Case III. For \left(\iota_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{2}, it is assumed that \iota_{4} and \iota_{3} \notin \mathscr{E} without loss of generality. Case III-1. If \pm \sqrt{\zeta_{l_{3}}} \pm \sqrt{\zeta_{l_{4}}}=0, then \left|h_{l_{1} l_{2} l_{3} l_{4}, k}\right|=|<k, \omega>\pm \sqrt{\zeta_{l_{1}}} \pm \sqrt{\zeta_{l_{2}}}|, Assuming that \Omega^{2,1}=\cup_{|k| \geq 1} \bigcup_{\iota_{3}, \iota_{4} \in \mathscr{J}, \iota_{1}, l_{2} \in \mathcal{J}, \pm \sqrt{\zeta_{l_{3}}} \pm \sqrt{\zeta_{l_{4}}}=0} R_{l_{1} l_{2} l_{3} l_{4}, k} Then, we have \quad Measure \Omega^{2,1} \leq C \sum_{|k| \geq 1} \frac{\eta^{2} \delta \overline{3}}{|k|^{4}|k|}\left(n_{2}-n_{1}+1\right)^{2} \leq C \eta^{2} \delta^{\frac{1}{3}}\left(n_{2}-n_{1}+\right.1)^{2} \sum_{|k| \geq 1} \frac{1}{|k|^{5}} \leq C \eta^{2} \delta^{\frac{1}{3}}\left(n_{2}-n_{1}+1\right)^{2} \sum_{l \geq 1} 2^{2} l_{l^{5}}^{1} \leq C \eta^{2} \delta^{\frac{1}{3}} where the constant C depends on n_{1}, n_{2} and \eta. Case III-2. If \pm \sqrt{\zeta_{l_{3}}} \pm \sqrt{\zeta_{l_{4}}} \neq 0, then \iota_{3}-\iota_{4} \neq 0. Without loss of generality, it is assumed that l_{3}>l_{4} . Thus, l_{3}-\iota_{4} :=t_{0} \geq 1. Moreover, | \pm \sqrt{\zeta_{t_{3}}} \pm \sqrt{\zeta_{t_{4}}}| \geq \iota_{3}^{2}-\iota_{4}^{2}=\left(\iota_{3}-\iota_{4}\right)\left(\iota_{3}+\iota_{4}\right)=t_{0}\left(2 \iota_{4}+t_{0}\right) (3.7) If \iota_{4}>\widetilde{K} :=\eta|k|+n_{2}^{2}, it can be derived that | \pm \sqrt{\zeta_{\iota_{3}}} \pm \sqrt{\zeta_{\iota_{4}}}| \geq 2 \iota_{4}+t_{0}>2 \widetilde{K}+1 . since

$|<k, \omega>\pm \sqrt{\zeta_{\iota_{1}}} \pm \sqrt{\zeta_{l_{2}}}| \leq 2 \eta|k|+2 n_{2}^{2}$        (3.8)

and

$\left|h_{l_{1} \iota_{2} l_{3} l_{4}, k}\right| \geq| \pm \sqrt{\zeta_{l_{3}}} \pm \sqrt{\zeta_{l_{4}}}|-|<k, \omega>\pm \sqrt{\zeta_{l_{1}}} \pm \sqrt{\zeta_{l_{2}}}|$           (3.9)

$\left|h_{t_{1} t_{2} t_{3} t_{4}, k}\right|>2 \widetilde{K}+1-2 \eta|k|-2 n_{2}^{2}=1>C \frac{\eta^{2} \delta^{\frac{1}{3}}}{|k|^{4}}$

is true if $\delta$ is sufficiently small. Hence, it only needs to analyse $1 \leq \iota_{4} \leq \tilde{K} .$ If t_{0}>\tilde{K}+1, it can be deduced from (3.7) that | \pm \sqrt{\zeta_{t_{3}}} \pm \sqrt{\zeta_{t_{4}}}| \geq 2 t_{0_{4}}+t_{0}^{2}>2 t_{0}=2 \widetilde{K}+2. It follows from (3.8) and (3.9) that \left|h_{l_{1} l_{2} l_{3} l_{4}, k}\right| \geq 2 \widetilde{K}+2-2 \eta|k|-2 n_{2}^{2}=2 \eta|k|+2 n_{2}^{2}+2-2 \eta|k|-2 n_{2}^{2}=2>\frac{\eta^{2} \delta^{\frac{1}{3}}}{|k|^{4}}, as \delta is sufficiently small. Thus, it is necessary to study the case 1 \leq t_{0} \leq \widetilde{K}+1. Thus, 1 \leq \iota_{3}=\iota_{4}+t_{0} \leq 2 \widetilde{K}+2 . Assuming that \Omega^{2,2}=U_{|k| \geq 1} \bigcup_{l_{4}, l_{3} \in \mathscr{Z}, \iota_{1}, l_{2} \in \mathcal{J}, \pm} \sqrt{\zeta_{l_{3}} \pm \sqrt{\zeta_{l_{4}}} \neq 0} R_{l_{1} l_{2} l_{3} l_{4}, k}, then we have Measure \Omega^{2,2} \leq C \sum_{|k| \geq 1} \frac{\eta^{2} \delta^{\frac{1}{3}}}{|k|^{4}|k|}\left(n_{2}-n_{1}+1\right)^{2}\left(\eta|k|+n_{2}^{2}\right)\left(2 \eta|k|+2 n_{2}^{2}+2\right) \leq C \eta^{2} \delta^{\frac{1}{3}}\left(n_{2}-n_{1}+1\right)^{2} \sum_{|k| \geq 1} \frac{1}{|k|^{5}}\left(n_{2}-n_{1}+1\right)^{2}\left(\eta|k|+n_{2}^{2}\right)\left(2 \eta|k|+2 n_{2}^{2}+2\right) \leq C \eta^{2} \delta^{\frac{1}{3}}\left(n_{2}-n_{1}+1\right)^{2} \sum_{l \geq 1} 2^{2} l^{2} \frac{1}{l^{3}} \leq C \eta^{2} \delta^{\frac{1}{3}}, where C is dependent of n_{1}, n_{2} and \eta . Thus, for \left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{2}, there exists a constant C satisfying Measure\Omega ^{2} \leq C \eta^{2} \delta^{\frac{1}{3}} . To sum up, assuming \overline{\Omega}=[\eta, 2 \eta]^{2} \backslash \tilde{\Omega}, meas \overline{\Omega} \geq\left(1-C_{2} \delta^{\frac{1}{3}}\right) \eta^{2} is valid, where the constant C_{2} is dependent of n_{1}, n_{2} and \eta . Proposition 3.1 Concerning the Hamiltonian (3.1), if parameter δ is sufficiently small for each index set \mathscr{E}, then there is a subset \Omega \subset[\eta, 2 \eta]^{2} satisfying Measure \Omega> 0 such that for each \omega \in \Omega, there exists a transformation \gamma that changes (3.1) to \mathbf{a} normal form, H^{\circ} \Upsilon=\Lambda+\delta \overline{G}+\delta \hat{G}+\delta^{2} K where \overline{G}(z, \overline{z})=\frac{1}{2} \sum_{\iota_{1} \in \mathcal{J}} or \iota_{2} \in \mathcal{J}_{l_{1}} \iota_{2}\left|Z_{l_{1}}\right|^{2}\left|Z_{l_{2}}\right|^{2} (3.10) \overline{G}_{\iota_{1} \iota_{2}}=\left\{\begin{array}{c}{\frac{3 \psi_{0}}{2 \pi \iota_{1}^{2} t_{2}^{2}}, l_{1} \neq l_{2}} \\ {\frac{9 \psi_{0}}{8 \pi \iota_{1}^{2} t_{2}^{2}},=l_{2}}\end{array}\right. \hat{G}=\sum_{\left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{3}, l_{1} \pm l_{2} \pm l_{3} \pm l_{4}=0} \psi_{l_{l} l_{2} l_{3} l_{4}}\left(z_{l_{1}}+\overline{z}_{l_{1}}\right)\left(z_{l_{2}}+\overline{z}_{l_{2}}\right)\left(z_{l_{3}}+\overline{z}_{l_{3}}\right)\left(z_{l_{4}}+\right.\left.\overline{z}_{l_{4}}\right)+\sum_{|k| \geq 1} e^{i<k, \vartheta>} \sum_{\left(l_{1}, l_{2}, l_{3}, l_{4}\right) \in \Delta_{3}} \psi_{k, l_{1} l_{2} l_{3} l_{4}}\left(z_{t_{1}}+\overline{z}_{t_{1}}\right)\left(z_{t_{2}}+\overline{z}_{t_{2}}\right)\left(z_{t_{3}}+\overline{z}_{t_{3}}\right)\left(z_{t_{4}}+\overline{z}_{t_{4}}\right) (3.11) and \delta^{\frac{1}{3}}|K|=\mathcal{O}\left(\left(\|z\|_{a, s}\right)^{6}\right) . The transformation is real analytic and canonical. Besides, \Upsilon is well defined in D_{1}\left(\frac{\sigma_{1}}{2}\right) \times u, with \mathcal{U} \subset l^{a, s} being a neighbourhood of the origin. Proof Let z_{j}=w_{j}, \overline{z}_{j}=w_{-j}(j \geq 1) and w_{0}=0 . Then, we have H=<\omega, J>+\sum_{j \geq 1} \sqrt{\zeta_{j}} w_{j} w_{-j}+\delta \sum_{l_{1}, l_{2}, l_{3}, l_{4},\left|l_{1}\right| \pm\left|l_{2}\right| \pm\left|l_{3}\right| \pm\left|l_{4}\right|=0} \psi_{l_{1} l_{2} l_{3} l_{4}} w_{l_{1}} w_{l_{2}} w_{l_{3}} w_{l_{4}} +\delta \sum_{|k| \geq 1} \sum_{\iota_{1}, l_{2}, l_{3}, l_{4}} \psi_{k, \iota_{1} \iota_{2} l_{3} l_{4}} e^{i<k, \vartheta>} w_{l_{1}} w_{l_{2}} w_{l_{3}} w_{l_{4}} where \iota_{1}, l_{2}, l_{3}, l_{4} \in \mathbb{Z} /\{0\} and \psi_{l_{1} l_{2} l_{3} l_{4}} :=\frac{G_{l_{1} l_{2} l_{3} l_{4}}}{16\left|\iota_{1} l_{2} l_{3} l_{4}\right|}, \psi_{k, l_{1} l_{2} l_{3} l_{4}} :=\frac{G_{k, l_{1} l_{2} l_{3} l_{4}}}{16\left|\iota_{1} l_{2} l_{3} l_{4}\right|} Clearly, \psi_{l_{1} l_{2} l_{3} l_{4}}=0 unless \left|\iota_{1}\right| \pm\left|\iota_{2}\right| \pm\left|\iota_{3}\right| \pm\left|\iota_{4}\right|=0 (3.12) Assuming that \mathcal{S}=\delta S=\delta S_{l_{1}, l_{2}, l_{3}, l_{4}} S_{l_{1} l_{2}} \iota_{3} \iota_{4} w_{l_{2}} w_{l_{2}} w_{l_{4}}+ \delta \sum_{|k| \geq 1} \sum_{l_{1}, l_{2}, l_{3}, l_{4}} S_{k, l_{1} l_{2} l_{3}} l_{4} e^{i<k, \vartheta>} w_{l_{1}} w_{l_{2}} w_{l_{3}} w_{l_{4}} with coefficients i S_{l_{1} l_{2} l_{3} l_{4}}=\left\{\begin{array}{l}{\frac{\psi_{t_{1} t_{2} t_{3} t_{4}}}{\xi_{t_{1}}+\xi_{t_{2}}+\xi_{t_{3}}+t_{t_{4}}}, \text { if }\left|t_{1}\right| \pm\left|t_{2}\right| \pm\left|t_{3}\right| \pm\left|t_{4}\right|=0 \text { and }\left|t_{1}\right|,\left|t_{2}\right|,\left|t_{3}\right|,\left|t_{4}\right| \in \overline{\overline{\Delta}}} \\ {0, \text { otherwise. }}\end{array}\right. and for k≠0, i S_{k, \iota_{1} l_{2} l_{3} l_{4}}=\left\{\begin{array}{c}{\frac{\psi_{k, l_{1} l_{2} l_{3} l_{4}}}{<k, \omega>},|k| \geq 1,\left|l_{1}\right|,\left|l_{2}\right|,\left|l_{3}\right|,\left|l_{4}\right| \in \overline{\Delta}, \text { and }} \\ {\zeta_{l_{1}}+\zeta_{l_{2}}+\zeta_{l_{3}}+\zeta_{l_{4}}=0} \\ {\zeta_{k_{1}, l_{2} l_{3} l_{4}}^{\prime+\zeta_{1}}|k| \geq 1, \quad\left|l_{1}\right|,\left|l_{2}\right|,\left|l_{3}\right|,\left|l_{4}\right| \in \overline{\Delta}, \text { and }} \\ {\zeta_{l_{1}}^{\prime+\zeta_{1},^{\prime}+\zeta_{l_{4}}^{\prime}+\zeta_{l_{4}}^{\prime}+<k, \omega>},|k| \geq 1, \quad\left|l_{1}\right|,\left|l_{2}\right|,\left|l_{3}\right|,\left|l_{4}\right| \in \overline{\Delta}, \text { and }} \\ {0, \text { otherwise }}\end{array}\right. where \zeta_{i^{\prime}}=\operatorname{sgni} \cdot|i|^{2}. For S_{l_{1} l_{2} l_{3} l_{4}}, the divisor \left|\zeta_{l_{1}}+\zeta_{l_{2}},+\zeta_{l_{3}},+\zeta_{l_{4}}^{\prime}\right| \geq 1 for all (|i|,|j|,|d|,|l|) \in \overline{\overline{\Delta}} according to the definition of admissible set. Lemma 3.1 in Wang et a l .(2018) shows that there exists a subset \Omega \subset[\eta, 2 \eta]^{2} such that, for all 0 \neq k \in \mathbb{Z}^{2}, any \omega \in \Omega satisfies |<k, \omega>| \geq \frac{\eta \delta^{\frac{1}{3}}}{|k|^{4}} and Measure \underline{\Omega} \geq\left(1-C_{1} \delta^{\frac{1}{3}}\right) \eta^{2}, where the constantC_{1} is an absolute constant. Considering Lemma 3.1, it is assumed that \Omega=\overline{\Omega} \cap \Omega . Thus, Measure \Omega \geq \eta^{2}\left(1-C \delta^{\frac{1}{3}}\right) is valid and Measure \Omega>0 as \delta sufficiently small. Using the same proof for Proposition 3.1 in Wang et al. (2018), it can be proved that the vector-field of X_{S} is real analytic in some complex neighbourhood \vartheta \in D_{1}\left(\frac{\sigma_{1}}{2}\right) of \mathbb{T}^{2} and a neighbourhood of the origin in l^{a, s} . Moreover, \left\|\frac{\partial S}{\partial w}\right\|_{a, S} \leq \frac{C}{2^{3}}\left(\|w\|_{a, S}\right)^{3} is true. Let Y=X_{\mathcal{S}}^{1} be the time-one map of vector field, then Y satisfies the result of this theorem. Other estimates can be found in Proposition 3.1 in Wang et al. (2018) . Q.E.D. 4. Conclusions Let \zeta_{j} \in[0,1] and \mathbb{Z}_{1} :=\mathbb{Z}^{+} \backslash \mathscr{L} . Under the complex coordinates \left\{\begin{array}{l}{z_{n_{1}}=\sqrt{\zeta_{1}+I_{1}} e^{-i \theta_{1}}} \\ {z_{n_{2}}=\sqrt{\zeta_{2}+I_{2}} e^{-i \theta_{2}}} \\ {z_{j}=w_{j}, j \in \mathbb{Z}_{1}}\end{array}\right. (4.1) the Hamiltonian can be transformed into. H=\sum_{1 \leq i \leq 2} \omega_{i} J_{i}+\sum_{1 \leq j \leq 2} \varpi_{j} I_{j}+\sum_{l \in \mathbb{Z}_{1}} \widehat{\Omega}_{l} w_{l} \overline{w}_{l}+P. (4.2) The corresponding symplectic structure becomes \sum_{1 \leq i \leq 2} d \vartheta_{i} \wedge d J_{i}+ \sum_{1 \leq j \leq 2} d \theta_{j} \wedge d I_{j}+i \sum_{l \in Z_{1}} d w_{l} \wedge d \overline{w}_{l}, \quad where P=\delta \overline{G}+\delta \hat{G}+\delta \hat{G}+\delta^{2} K, with \overline{G}= \frac{1}{2} \sum_{1 \leq i, j \leq 2} \overline{G}_{n_{i} n_{j}}\left(I_{i}+\zeta_{i}\right)\left(I_{j}+\zeta_{j}\right)+\sum_{l \in Z_{1}, 1 \leq l \leq 2} \overline{G}_{l n_{j}}\left(I_{j}+\zeta_{j}\right)\left|w_{l}\right|^{2}, \quad \varpi=\alpha+\delta \tilde{A}_{S} \hat{\Omega}=\zeta+\delta B \zeta, \alpha=\left(\sqrt{\zeta}_{n_{1}}, \sqrt{\zeta}_{n_{2}}\right), \zeta=(\sqrt{\zeta_{l}})_{l \in \mathbb{Z}_{1}}, and \tilde{A}=\left(\begin{array}{cc}{\overline{G}_{n_{1} n_{1}}} & {\overline{G}_{n_{1} n_{2}}} \\ {\overline{G}_{n_{2} n_{1}}} & {\overline{G}_{n_{2} n_{2}}}\end{array}\right), B=\left(\begin{array}{ccc}{\overline{G}_{1 n_{1}}} & {\overline{G}_{1 n_{2}}} \\ {\overline{G}_{2 n_{1}}} & {\overline{G}_{2 n_{2}}} \\ {\vdots} & {\vdots} \\ {\overline{G}_{l n_{1}}} & {\overline{G}_{l n_{2}}} \\ {\vdots} & {\vdots}\end{array}\right)_{l \in \mathbb{Z}_{1}} Assuming that \omega=\omega_{-}+\delta^{\frac{3}{2}} \overline{\omega}, \overline{\omega} \in[0,1]^{2}, where \omega_{-} \in \Omega is fixed and \omega \in \overline{\Omega} :=\left\{\omega \in \Omega| | \omega-\omega_{-} | \leq \delta^{\frac{3}{2}}\right\}, it is clear that \overline{\overline{\Omega}} \times[0,1]^{2} \subset \Omega \times[0,1]^{2} Then, the variables were scaled by setting \overline{\omega}=\delta^{\frac{1}{2}} \widetilde{\omega}, \zeta=\delta^{\frac{1}{2}} \tilde{\zeta}, w=\delta^{\frac{1}{4}} \widetilde{w}, \overline{w}=\delta^{\frac{1}{4}} \widetilde{w}, I=\delta^{\frac{1}{2}} \tilde{I}, and J=\delta^{\frac{1}{2}} \tilde{\jmath} . The scaled Hamiltonian can be expressed as: \begin{aligned} \widetilde{H} &=\delta^{-\frac{3}{2}} H\left(\vartheta, \delta^{\frac{1}{2}} \tilde{J}, \theta, \delta^{\frac{1}{2}} \tilde{I}, \delta^{\frac{1}{4}} \widetilde{W}, \delta^{\frac{1}{4}} \widetilde{W}, \delta^{\frac{1}{4}} \widetilde{\omega}, \delta^{\frac{1}{4}} \tilde{\zeta}\right)=\sum_{1 \leq i \leq 2} \widetilde{\omega}_{i} \tilde{J}_{i}+\sum_{1 \leq l \leq 2} \widetilde{\varpi}_{l} \tilde{I}_{l}+\\ \sum_{j \in Z_{1}} \tilde{\Omega}_{j} \tilde{w}_{j} \tilde{w}_{j}+\tilde{P} & \end{aligned} where \widetilde{\omega}_{1}(\widetilde{\omega})=\delta^{-1} \omega_{-1}+\delta \widetilde{\omega}_{1}, \quad \widetilde{\omega}_{2}(\widetilde{\omega})=\delta^{-1} \omega_{-2}+\delta \widetilde{\omega}_{2}, \quad \widetilde{\omega}(\widetilde{\omega})=\left(\widetilde{\omega}_{1}(\widetilde{\omega}), \widetilde{\omega}_{2}(\widetilde{\omega})\right), \widetilde{\varpi}(\zeta)=\delta^{-1} \alpha+\delta^{\frac{1}{2}} \tilde{A} \tilde{\zeta}, and \widehat{\Omega}(\zeta)=\delta^{-1} \zeta+\delta^{\frac{1}{2}} B \tilde{\zeta} . It is clear that \omega=\delta \widetilde{\omega}, \varpi=\delta \widetilde{\varpi}, and \widehat{\Omega}=\delta \tilde{\widehat{\Omega}} . Then, some notations were introduced as \widehat{\omega}_{1}=\widetilde{\omega}_{1}(\widetilde{\omega}), \quad \widehat{\omega}_{2}=\widetilde{\omega}_{2}(\widetilde{\omega})\widetilde{\varpi}_{1}(\tilde{\zeta}), \widetilde{\varpi}_{2}(\tilde{\zeta}) ; \widehat{\omega}=(\widetilde{\omega}(\widetilde{\omega}), \widetilde{\varpi}(\tilde{\zeta})) ; \xi=(\widetilde{\omega}, \tilde{\zeta}) \in \Pi ; \Pi=[\beta, 2 \beta] ; and $\beta=\delta^{-\frac{1}{3}} .$ Let $\sigma_{0}=\frac{\sigma_{1}}{2}$ and $r=r_{0},$ where $0<r_{0}<1$ and $r_{0}$ is a constant. Let $\sigma=\min \left\{\frac{\sigma_{0}}{2}, \frac{1}{2}\right\}$$M_{11}=1, M_{12}=\frac{21\left|\psi_{0}\right|}{32 \pi}, M_{2}=\frac{3\left|\psi_{0}\right|}{2 \pi}, M=\max \left\{M_{11}+M_{12}, M_{2}\right\}, \tau>9, \mu=2 \tau+3$$\gamma_{0} \leq \frac{1}{c(M+1) 2^{6+4 \mu}}$ and $\gamma=\frac{\gamma_{0}^{6}}{20^{2(1+\mu)(c M)^{6}}} .$ Note that $M$ does not depend on $\delta .$

For a function $Q,$ the corresponding Hamiltonian vector field can be defined as

$X_{Q}=\left(Q_{\tilde{\jmath}},-Q_{\vartheta}, Q_{\tilde{I}},-Q_{\theta}, i Q_{\tilde{w}},-i Q_{\tilde{w}}\right)^{T},$

and the weighted norm for $X_{Q}$ can be defined as:

$\left|X_{Q}\right|_{r, n}^{*}=\frac{1}{r^{2}}\left\|Q_{\vartheta}\right\|_{\Pi}^{*}+\frac{1}{r^{2}}\left\|Q_{\theta}\right\|_{\Pi}^{*}+\left\|Q_{\overline{I}}\right\|_{\Pi}^{*}+\frac{1}{r}\left\|Q_{\widetilde{w}}\right\|_{a, S, \Pi}^{*}+\frac{1}{r}\left\|Q_{\tilde{w}}\right\|_{a, S, \Pi}^{*}$

where

$\|Q\|_{\Pi}^{*}=\max \left\{\sup _{\xi \in \Pi}|Q|, \sup _{\xi \in \Pi}\left|\frac{\partial Q}{\partial \xi}\right|\right\}$

Taking $\delta \leq\left(\frac{\gamma_{0}^{6}}{2020(1+\mu)(c M)^{6}} \sigma^{2 \mu+3}\right)^{2}$ and using the same proof for Theorem 4.1 in Wang et al. $(2018),$ it can be derived that there exists a set $\widetilde{\Pi}_{\delta} \subset \Pi$ , a family of torus embedding $\Phi : \mathbb{T}^{4} \times \widetilde{\Pi}_{\delta} \rightarrow \mathcal{P} a, s$ and a map $\widetilde{\widetilde{\omega}}_{0}=\left(\widetilde{\omega}_{0}, \widetilde{\varpi}_{0}\right) : \widetilde{\Pi}_{\delta} \rightarrow \mathbb{R}^{4}$ . that satisfy the following conditions: for any $\xi \in \widetilde{\Pi}_{\delta},$ the map $\Phi$ restricted to $\mathbb{T}^{4} \times\{\xi\}$ is a real analytic embedding of a rotational torus, whose frequency vector is $\widetilde{\omega}_{0}(\xi)$ for $H$ at $\xi$ ;$\widetilde{\Pi}_{\delta}$ is a Cantor set, and $\Phi, \widetilde{\widetilde{\omega}}_{0}$ are Whitney smooth; every embedding is real analytic in $|\operatorname{Im} \vartheta|<\frac{\sigma}{2}$ and $|\operatorname{Im} \theta|<\frac{\sigma}{2} ;\left|\Phi-\Phi_{0}\right|_{r}^{*} \leq c \delta^{\frac{1}{4}}$ and $\left\|\widetilde{\widetilde{\omega}}_{0}-\widehat{\omega}\right\|^{*} \leq c \delta^{\frac{1}{2}}$ hold uniformly, where $\Phi_{0}$ is the trivial embedding.

Returning $\tilde{\Pi}_{\delta}$ to the subset in $\overline{\Omega} \times[0,1]^{2},$ namely $\Sigma_{\delta}$ , there exists a Cantor set

$\Sigma_{\delta} \subset \Omega \times[0,1]^{2}$ satisfying the result in the following Theorem $4.1 .$ Returning $\widetilde{\omega}_{0}$ to the frequencies in the system with Hamiltonian $(4.2),$ namely $\widehat{\omega}_{0},$ the frequency vector can be estimated. Therefore, the nonlinear equation $(1.1)$ admits a Cantor family of rotational tori, which are 4 -dimensional. Their frequency vectors are $\widehat{\omega}_{0}=\left(\omega_{01}, \omega_{02}, \varpi_{0 n_{1}}, \varpi_{0 n_{2}}\right),$ where $\omega_{01}=\omega_{1}+\mathcal{O}(\delta), \omega_{02}=\omega_{2}+\mathcal{O}(\delta), \varpi_{0 n_{1}}=\zeta_{n_{1}}+$$\mathcal{O}(\delta),$ and $\varpi_{0 n_{2}}=\zeta_{n_{2}}+\mathcal{O}(\delta) .$ A big part of the family of tori persists under small perturbations and is linearly stable. The quasi-periodic solutions have small amplitudes and zero Lyapunov exponents. In short, the following theorem is valid.

Theorem 4.1 Assuming that (A1), (A2) and (A3) are valid, for every admissible index set $\mathscr{E} :=\left\{\left(n_{1}, n_{2}\right) | n_{1}, n_{2} \text { are odd, } n_{1} \neq 7 \bmod (14), n_{2}>6 n_{1}^{2}\right\},$ there exits a $\delta^{*}$ which satisfies the following condition: for $0<\delta<\delta^{*},$ there exist sets $\Omega \subset$ $[\eta, 2 \eta]^{2}$ and $\Sigma_{\delta} \subset \Sigma :=\Omega \times[0,1]^{2}$ such that for any $\xi=\left(\omega_{1}, \omega_{2}, \zeta_{n_{1}}, \zeta_{n_{2}}\right) \in \Sigma_{\delta}$ Equation $(1.1)$ under the conditions $(1.2)$ has a quasi-periodic solution.

$u(t, x)=\frac{2}{n_{1}} \sqrt{\frac{\zeta n_{1}+O\left(\delta^{\frac{1}{4}}\right)}{\pi}} \sin n_{1} x \cos \varpi_{0 n_{1}}(\xi) t+\frac{2}{n_{2}} \sqrt{\frac{\zeta_{n_{2}}+O\left(\delta^{\frac{1}{4}}\right)}{\pi}} \sin n_{2} x \cos w_{0 n_{2}}(\xi) t+\mathcal{O}\left(\delta^{\frac{1}{4}}\right)$,

where

$\left|\varpi_{0 j}-j^{2}\right| \leq c \delta, \Omega$ and $\Sigma_{\delta}$  have positive Lebesgue measures.

Les différentes sections sont numérotées de l’introduction jusqu’à la conclusion. Les remerciements et la bibliographie (ainsi que l’extended abstract) ne sont pas numérotés. Les intertitres sont alignés à gauche sans alinéa, comme suit. Les espaces au-dessus s’annulent quand ils sont précédés par un autre inter.

Acknowledgement

This work is supported by NNSFC (Nos. 11601270, 11701567, 11501571).

References

Cao C., Yuan X. (2017). Quasi-periodic solutions for perturbed generalized nonlinear vibrating string equation with singularities. Discrete & Continuous Dynamical Systems - Series A, Vol. 37, No. 4, pp. 1867-1901. https://doi.org/10.3934/dcds.2017079

Chen B. B., Fu Z. H., Chen T. (2017). Stability analysis and evaluation of a landslide area in Sichuan. Environmental and Earth Sciences Research Journal, Vol. 4, No. 2, pp. 49-54. https://doi.org/10.18280/eesrj.040205

Chen B. B. (2017). Finite element strength reduction analysis on slope stability based on ANSYS. Environmental and Earth Sciences Research Journal, Vol. 4, No. 3, pp. 60-65. https://doi.org/10.18280/eesrj.040302

Eliasson L. H., Grébert B., Kuksin S. B. (2016). KAM for the nonlinear beam equation. Geometric and Functional Analysis, Vol. 26, pp. 1588-1715. https://doi.org/10.1007/s00039-016-0390-7

Gao M., Liu J. (2017). Invariant tori for 1D quintic nonlinear wave equation. Journal of Differential Equations, Vol. 263, No. 12, pp. 8533-8564. https://doi.org/10.1016/j.jde.2017.08.057

Ge C., Geng J. (2018). KAM tori for higher dimensional quintic beam equation. Journal of Dynamics and Differential Equations, Vol. 2018, pp. 1-15. https://doi.org/10.1007/s10884-018-9661-3

Geng J., You J. (2003). KAM tori of Hamiltonian perturbations of 1D linear beam equations. J. Math. Anal. Appl., Vol. 277, pp. 104-121. https://doi.org/10.1016/s0022-247x(02)00505-x

Geng J., You J. (2006). KAM tori for higher dimensional beam equations with constant potentials. Nonlinearity, Vol. 19, pp. 2405-2423. https://doi.org/10.1088/0951-7715/19/10/007

Geng J., Zhou S. (2018). An infinite dimensional KAM theorem with application to two dimensional completely resonant beam equation. Journal of Mathematical Physics, Vol. 59, No. 7, pp. 072702. https://doi.org/10.1063/1.5045780

Liang Z., Geng J. (2006). Quasi-periodic solutions for 1D resonant beam equation. Communications on Pure and Applied Analysis, Vol. 5, No. 4, pp. 839-853. https://doi.org/10.3934/cpaa.2006.5.839

Liu J., Yuan X. (2014). KAM for the derivative nonlinear Schrödinger equation with periodic boundary conditions. Journal of Differential Equations, Vol. 256, No. 4, pp. 1627-1652. https://doi.org/10.1016/j.jde.2013.11.007

Liu W., Xue Y. J. (2017). A static load test study for one continuous beam bridge. Environmental and Earth Sciences Research Journal, Vol. 4, No. 4, pp. 87-92. https://doi.org/10.18280/eesrj.040401

Procesi M. (2010). A normal form for beam and non-local nonlinear Schrödinger equation. Journal of Physics A: Mathematical and Theoretical, Vol. 43, pp. 434028. https://doi.org/10.1088/1751-8113/43/43/434028

Si W., Si J. (2017). Linearization of a quasi-periodically forced flow on, under Brjuno–Rüssmann non-resonant condition. Applicable Analysis, Vol. 2017, pp. 1-24. https://doi.org/10.1080/00036811.2017.1350847

Si W., Si J. (2018). Elliptic-type degenerate invariant tori for quasi-periodically forced four-dimensional non-conservative systems. Journal of Mathematical Analysis & Applications, Vol. 460, No. 1, pp. 164-202. https://doi.org/10.1016/j.jmaa.2017.11.047

Tuo Q., Si J. (2015). Quasi-periodic solutions of nonlinear beam equations with quintic quasi-periodic nonlinearities. Electronic Journal of Differential Equations, Vol. 2015, pp. 1-20.

Wang Y., Liu J., Zhang M. (2018). Quasi-periodic solutions for a Schrödinger equation with a quintic nonlinear term depending on the time and space variables. Boundary Value Problems, Vol. 2018, No. 1, Article: 76, pp. 1-30. https://doi.org/10.1186/s13661-018-0996-9