A Nonlinear Schrödinger Model for Many-Particle Quantum Systems

Abstract

Considering both effects of the s-wave scattering and the atom-atom interaction rather than only the effect of the s-wave scattering, we establish a nonlinear Schrödinger model for many-particle quantum systems and we prove the global existence of a solution to the model and obtain the expression of the solution. Furthermore, we show that the Hamilton energy and the total particle number both are conservative quantities.

1. Introduction

As the fundamental equations in quantum mechanics, nonlinear Schrödinger (NLS) equations are usually chosen as models to describe many different kinds of many-particle quantum systems. One of the most typical examples is the Gross-Pitaevskii (GP) equation [1, 2] which was derived from a mean field approximation and used to describe the Bose-Einstein condensates (BEC) [3–7] for trapped dilute-gas at zero temperature.

GP-equation has been extensively studied during the past decades [8–12]. Numerical analyses have been applied to GP-equation to investigate the dynamics of BEC [8, 9]; analytical methods have also been used for solving the GP-equation to predict properties of the condensates [10], and rigorous mathematical proof has been provided to guarantee the existence of travelling wave solutions to the GP-equation [11, 12].

Apart from these studies, work related with utilizing the generalized GP-equation to investigate physical phenomena still attracts much attention [13–16]. Coste [13] derived a generalized GP-equation from the correction for the Lagrangian of the original GP-model and this model can describe both the two-fluid model and the Hills-Roberts model under two circumstances. By particle-number-conserving Bogoliubov method, Gardiner [14] demonstrated the validity of the time-dependent GP-equation for a highly condensed Bose gas. And with an equivalent method, Castin and Dum [15] obtained a generalized GP-equation which can yield both the time-dependent GP-equation for the condensate wave function and the linear dynamics of noncondensed particles in two situations. Furthermore, building on the works of Gardiner [14] and Castin and Dum [15], Gardiner and Morgan [16] derived a generalized GP-equation which can describe the condensate and noncondensate dynamics of Bose-Einstein dilute atomic gas at finite temperature.

Similarly, in this paper, we also acquire a generalized GP-equation. In the following we will outline the aim of this work.

It is well known that GP-equation has a wide range of validity provided that the scattering length (denoted by 𝑎) is much smaller than the average distance between particles (denoted by 𝑑). In the repulsive case [3, 4], from the physics point of view, the atom-atom interaction is effectively weak and dominated by the s-wave scattering, so the realistic interaction between particles can be well approximated by the s-wave scattering [17]. On the other hand, from the mathematics point of view, the solution to GP-equation is well defined in the repulsive case (i.e., 𝑎>0) since there exists only one global solution to GP-equation; see [18–24] for more detail.

However, GP-equation is not consistent very well with the attractive case [4]. For the attractive case (i.e., 𝑎<0), blow-up (collapse) may take place in the 2D and 3D cases, see [25–30]. In fact, as the temperature approaches to zero, the kinetic energy be small, which implies that blow-up deduced mathematically from GP-equation never happens in the experiments. Therefore, GP-model is not a correct model for describing the attractive case since it violates the compatibility of physical fact and mathematical result. To give a reasonable model which is compatible with physical fact and mathematical result is one of the motivations for this manuscript.

And to give a model which includes both effects of the s-wave scattering and the atom-atom interaction to describe more general many-particle quantum system near zero temperature is another motivation for this manuscript. It is noted that the atom-atom interaction can not be neglected when the scattering length is not much smaller than the average distance between particles. In this situation, GP-equation is not a good model to describe general many-particle quantum system.

In this paper, we establish an NLS model for more general many-particle quantum systems. Different from the interactions considering in GP-equation, the interactions among particles in the NLS model include both the s-wave scattering and the atom-atom interaction. And we will see later (Theorem 3.1) that there exists a global solution for the NLS model and no blow-up takes place. Furthermore, we will show that the NLS model can be regarded as a generalization of GP-equation. In the end, we prove that the Hamilton energy and the total particle number both are conservative quantities.

This paper is organized as follows. Section 2 derives the new Hamilton energy from the correction of the original one and obtains the NLS model. Section 3 proves rigorously the global existence of solution to the model and obtains the expression of the solution. Section 4 verifies that the conservation laws hold true. Section 5 discusses some existing approaches and compares them with ours. And Section 6 is devoted to the conclusions.

2. The NLS Model for Many-Particle Quantum Systems

In order to obtain the NLS model, we take two steps. At first, we derive the new Hamilton energy from the correction of the original one. And then the NLS model can be obtained by applying the theory of quantum physics to the Hamiltonian.

At first, we recall the original GP-equation as follows: 𝑖ℏ𝜕𝜓ℏ𝜕𝑡=−²(𝑥)𝜓2𝑚Δ𝜓+𝑉𝜓+𝑈²𝜓, (2.1) where 𝑚 the boson mass, ℏ Planck constant, 𝑉(𝑥) the external trapping potential, |𝜓|² the density of bosons, and 𝑈 the interaction “strength”, given by 𝑈=4𝜋𝑎ℏ²𝑚, (2.2) where 𝑎 is the s-wave scattering length with following physical interpretation: 𝑎>0,therepulsiveinteraction,<0,theattractiveinteraction. (2.3)

Also, we note that the corresponding Hamilton energy of (2.1) as follows: 𝐻𝜓=_Ωℏ²4𝑚∇𝜓²+12𝑉(𝑥)𝜓²+14𝑈𝜓⁴𝑑𝑥, (2.4) where the first term in (2.4), that is, _Ωℏ²4𝑚∇𝜓²𝑑𝑥, (2.5) represents the kinetic energy of bosons, the second term in (2.4), that is, _Ω12𝑉(𝑥)𝜓²𝑑𝑥, (2.6) represents the external trapping potential energy and the last term in (2.4), that is, _Ω14𝑈𝜓⁴𝑑𝑥, (2.7) represents the bosons interaction potential energy.

Since the physical interpretation of the kinetic energy (2.5) and the external trapping potential energy (2.6) of GP-equation are the same as those of the NLS model and the only difference between them is the interaction potential energy, the Hamilton energy of the NLS model can be expressed as follows: 𝐻𝜓=_Ωℏ²4𝑚∇𝜓²+12𝑉(𝑥)𝜓²+12𝑔𝜓²𝜓²𝑑𝑥, (2.8) where function 𝑔(⋅)∶𝑅⁺→𝑅 is a 𝐶¹ function undetermined. Some essential information of function 𝑔 can be derived from the following analysis.

For the NLS model, the interaction potential energy is built on the basis of the wave-particle duality in quantum mechanics, the assumptions that the atom-atom interaction be chosen to be the van der Waals force [31, 32], and the interaction potential energy is changed continuously with density of particles.

The wave-particle duality in quantum mechanics points out that the many-particle quantum system has both the properties of wave and particle, which implies that the interactions among particles include both of the s-wave scattering and the atom-atom interaction. The interaction mechanisms of the former are the same as wave but the mechanisms of the latter are the same as particle. More precisely, if the scattering length is much smaller than the average distance between particles (i.e., 𝑎≪𝑑), the s-wave scattering takes the leading role, and if the scattering length is much bigger than the average distance between particles (i.e., 𝑎≫𝑑), the atom-atom interaction plays dominant role, or else the two both work.

If the scattering length is much smaller than the average distance between particles (i.e., 𝑎≪𝑑), the realistic interaction between particles can be approximated by the s-wave scattering as shown in (2.7), then we can infer from (2.7) that 𝑔(𝑧) and 𝑧 follow the linear relationship, that is, 𝑔(𝑧)=𝑐₀𝑧, (2.9) for general many-particle quantum systems provided that 0≤𝑧≤𝜌₀, where 𝜌₀∈𝑅⁺ is sufficiently small constant since the trapped gas is dilute and 𝑐₀∈𝑅⁺ or 𝑐₀∈𝑅⁻ corresponds to repulsive and attractive case, respectively.

If the scattering length is much bigger than the average distance between particles (i.e., 𝑎≫𝑑), the atom-atom interaction is chosen to be the van der Waals interaction, see [31, 32] and the references therein and the relationship between the atom-atom interaction potential energy and the average distance between particles can be depicted as shown in the Figure 1.

Figure 1 

The atom-atom interaction potential energy as a function of the average distance between particles.

Since the average distance between particles and the density of particles are subject to conservation of mass, the relationship between them satisfies 𝜓²∝1𝑑³, (2.10) then together with Figure 1 the relationship between the atom-atom interaction potential energy and the density of particles can be derived as shown in the Figure 2.

Figure 2 

The atom-atom interaction potential energy as a function of the density of particles.

Combining relationship (2.9) with Figure 2, we can get the effects of the s-wave scattering and the van der Waals interaction as shown in the Figure 3; (0,𝜌₀) is the domain in which the s-wave scattering takes the leading role, (𝜌₁,𝜌₂) is the domain in which the van der Waals force plays the dominant role, and (𝜌₀,𝜌₁) is the domain in which the two both work.

Figure 3 

Effects of the s-wave scattering and the van der Waals interaction.

Considering both effects of the s-wave scattering and the van der Waals interaction and the assumption that the interaction potential energy is changed continuously with density of particles, we take function 𝑔 as shown in the Figure 4.

Figure 4 

Function 𝑔 for 𝑎.

Although the exact formula of 𝑔(𝑧) can not be obtained from Figure 4, noting the fact that the density of particles in experiments never is infinite and bounded above, that is, 𝜓²≤𝜌₂,𝜌₂∈𝑅⁺, (2.11) the following conditions hold true: 𝑔^′(𝑧)≤𝑐₁,0≤𝑧≤𝜌₂, (2.12) where 𝑐₁ is a positive constant and 𝑔(𝑧)=𝑐₀𝑧,0≤𝑧≤𝜌₀,𝑔₁(𝑧),𝜌₀<𝑧<𝜌₁,𝑔₂(𝑧),𝜌₁≤𝑧≤𝜌₂, (2.13) where 𝑔₁(𝑧), 𝑔₂(𝑧) are 𝐶¹ functions and 𝑔₂ satisfies 𝑐₂𝑧−𝑐₃≤𝑔₂(𝑧)≤𝑐₄𝑧−𝑐₅, (2.14) where 𝑐₂, 𝑐₃, 𝑐₄, 𝑐₅ are all positive constants.

The physical conditions (2.12) and (2.13) can be written as the following mathematical form: 𝑔^′(𝑧)≤𝑐₁𝑔(𝑧)=𝑐,∀𝑧≥0,₀𝑧,0≤𝑧≤𝜌₀,𝑔₁(𝑧),𝜌₀<𝑧<𝜌₁,𝑔₂(𝑧),𝑧≥𝜌₁, (2.15)(2.16) where 𝑔₁(𝑧), 𝑔₂(𝑧) are 𝐶¹ functions and 𝑔₂ satisfies 𝑐₂𝑧−𝑐₃≤𝑔₂(𝑧)≤𝑐₄𝑧−𝑐₅. (2.17)

According to the theory of quantum physics, that is, 𝑖ℏ𝜕𝜓=𝜕𝑡𝛿𝐻𝛿𝜓^∗, (2.18) we obtain the NLS model as follows: 𝑖ℏ𝜕𝜓ℏ𝜕𝑡=−²(𝑥)2𝑚Δ𝜓+𝑉𝜓+𝑔^′𝜓²𝜓²𝜓+𝑔𝜓²𝜓,𝜓|_𝜕Ω𝜓(0)=0,=𝜓₀=𝜙₁+𝑖𝜙₂, (2.19) where Ω be a bounded open set in 𝑅^𝑛(𝑛≤3) and (𝑥,𝑡)∈Ω×(0,∞).

Since |𝜓|²<𝜌₀ implies that the gas is dilute, the atom-atom interaction is effectively weak and the realistic interaction between particles can be approximated by the s-wave scattering. Under this condition and taking 𝑐₀=2𝜋𝑎ℏ²/𝑚 in (2.19), the NLS model (2.19) yields the GP-equation, which implies that (2.19) can be regarded as a generalization of the GP-equation.

3. Mathematical Results of the NLS Model

For the NLS model (2.19), we have the following global existence result.

Theorem 3.1. Assume that 𝑔 satisfies conditions (2.15), (2.16) and (2.17), if 𝑉(𝑥)∈𝐿²(Ω), then for any 𝜓₀∈𝐻¹(Ω,𝐶), there exists a global solution to (2.19) in 𝐶⁰([0,∞),𝐿²(Ω,𝐶))∩𝐿^∞((0,∞),𝐻¹(Ω,𝐶)). Furthermore, for all (𝑥,𝑡)∈Ω×[0,∞), the solution can be expressed as follows: 𝜓(𝑥,𝑡)=(cos𝑡𝐿+𝑖sin𝑡𝐿)𝜓₀−𝑖ℎ^𝑡₀[cos(𝑡−𝜏)𝐿+𝑖sin(𝑡−𝜏)𝐿]𝐺𝜓(𝑥,𝜏)𝑑𝜏, (3.1) where ℎ𝐿=12𝑚Δ−ℎ𝑉(𝑥)∶𝑋₁→𝑋^∗₁,𝐺𝜓=𝑔^′𝜓²𝜓²𝜓+𝑔𝜓²𝜓. (3.2)

Proof. Firstly, we prove the global existence of solution to (2.19) in 𝐿^∞((0,∞),𝐻¹(Ω,𝐶)) by Galerkin method.
Let 𝜓=𝑢₁+𝑖𝑢₂, by the theory of infinite dimensional Hamilton system proposed by Ma [24], (2.19) be equivalent to the following equations: 𝜕𝑢₁=𝑢𝜕𝑡𝛿𝐻₁,𝑢₂𝛿𝑢₂,𝜕𝑢₂𝑢𝜕𝑡=−𝛿𝐻₁,𝑢₂𝛿𝑢₁,𝑢_{𝑖∣𝜕Ω}𝑢=0,𝑖=1,2,_𝑖(0)=𝜙_𝑖,𝑖=1,2, (3.3) where 𝛿𝐻𝑢₁,𝑢₂𝛿𝑢₂ℏ=−2𝑚Δ𝑢₂+1ℏ𝑉(𝑥)𝑢₂+1ℏ𝑔^′𝑢²₁+𝑢²₂𝑢²₁+𝑢²₂𝑢₂+1ℏ𝑔𝑢²₁+𝑢²₂𝑢₂,𝛿𝐻𝑢₁,𝑢₂𝛿𝑢₁ℏ=−2𝑚Δ𝑢₁+1ℏ𝑉(𝑥)𝑢₁+1ℏ𝑔^′𝑢²₁+𝑢²₂𝑢²₁+𝑢²₂𝑢₁+1ℏ𝑔𝑢²₁+𝑢²₂𝑢₁. (3.4)
Let 𝑋₁∶=𝐻¹₀(Ω,𝑅²), 𝑋∶=𝐿²(Ω,𝑅²) and choose {𝑒_𝑘∣𝑘=1,2,…}⊂𝐻¹₀(Ω) as orthonormal basis of space 𝐿²(Ω).
Set 𝑋_𝑛, 𝑋_𝑛 as follows: 𝑋_𝑛=^𝑛_𝑘=1𝛼_𝑘𝑒_𝑘∣𝛼_𝑘,𝑋∈𝑅,1≤𝑘≤𝑛_𝑛=^𝑛_𝑘=1𝛽_𝑘(𝑡)𝑒_𝑘∣𝛽_𝑘(𝑡)∈𝐶¹[0,∞),1≤𝑘≤𝑛. (3.5)
Consider the ordinary equations as follows: 𝑑𝑥_𝑘(𝑡)=𝑢𝑑𝑡𝛿𝐻_𝑛,𝑣_𝑛𝛿𝑣_𝑛,𝑒_𝑘,𝑑𝑦_𝑘(𝑡)𝑢𝑑𝑡=−𝛿𝐻_𝑛,𝑣_𝑛𝛿𝑢_𝑛,𝑒_𝑘,𝑥_𝑘(0)=𝜙₁,𝑒_𝑘,𝑦_𝑘(0)=𝜙₂,𝑒_𝑘, (3.6) where 𝑢_𝑛=∑^𝑛_𝑘=1𝑥_𝑘(𝑡)𝑒_𝑘, 𝑣_𝑛=∑^𝑛_𝑘=1𝑦_𝑘(𝑡)𝑒_𝑘.
By the theory of ordinary equations, there exists only one local solution of (3.6): 𝑥₁(𝑡),𝑦₁(𝑡),…,𝑥_𝑛(𝑡),𝑦_𝑛(𝑡),0≤𝑡≤𝜏. (3.7)
From (3.6) we can obtain the equality 𝑢_𝑛,𝑢_𝑛+𝑣_𝑛,𝑣_𝑛=^𝑡₀𝛿𝐻𝑢_𝑛,𝑣_𝑛𝛿𝑣_𝑛,𝑢_𝑛−𝛿𝐻𝑢_𝑛,𝑣_𝑛𝛿𝑢_𝑛,𝑣_𝑛𝑑𝑡+𝜙^𝑛₁,𝑢_𝑛+𝜙^𝑛₂,𝑣_𝑛, (3.8) which holds true for any 𝑢_𝑛,𝑣_𝑛∈𝑋_𝑛, where 𝜙^𝑛₁=^𝑛_𝑘=1𝜙₁,𝑒_𝑘𝑒_𝑘,𝜙^𝑛₂=^𝑛_𝑘=1𝜙₂,𝑒_𝑘𝑒_𝑘. (3.9)
Moreover, equality ^𝑡₀𝑑𝑢_𝑛,𝑢𝑑𝑡^𝑛+𝑑𝑣_𝑛,𝑣𝑑𝑡^𝑛𝑑𝑡=^𝑡₀𝛿𝐻𝑢_𝑛,𝑣_𝑛𝛿𝑣_𝑛,𝑢_𝑛−𝛿𝐻𝑢_𝑛,𝑣_𝑛𝛿𝑢_𝑛,𝑣_𝑛𝑑𝑡 (3.10) holds true for any 𝑢_𝑛,𝑣_𝑛∈𝑋_𝑛.
Put (𝑢_𝑛,𝑣_𝑛)=(𝑑𝑣_𝑛/𝑑𝑡,−𝑑𝑢_𝑛/𝑑𝑡) into (3.10), we obtain that 0=^𝑡₀𝑑𝐻𝑢_𝑛,𝑣_𝑛𝑑𝑡𝑑𝑡, (3.11) which implies 𝐻𝑢_𝑛,𝑣_𝑛=𝐻𝜙^𝑛₁,𝜙^𝑛₂. (3.12)
Next, we claim that 𝐻𝑢₁,𝑢₂≥𝐶𝑢₁,𝑢_2𝑋1−𝐶. (3.13)
Since (2.16) and (2.17) holds true; we have the following result: lim_{|𝜓|2→+∞}𝑔𝜓²=+∞, (3.14) then there exists a positive number 𝜌₃, such that 𝑔𝜓²>0,∀𝜓²>𝜌₃. (3.15)
If |𝜓|²>𝜌₃, by Poincaré’s inequality and Young’s inequality (3.13) holds true; on the other hand, if |𝜓|²≤𝜌₃, then ∫_Ω(1/2ℎ)𝑔(|𝜓|²)|𝜓|²𝑑𝑥 be bounded below, by Poincaré’s inequality and Young’s inequality (3.13) also holds true.
Since (3.12) and (3.13) hold true, then {(𝑢_𝑛,𝑣_𝑛)} is bounded in 𝐿^∞((0,∞),𝑋₁). Therefore there exists a subsequence, we still write it as {(𝑢_𝑛,𝑣_𝑛)}^∞_𝑛=1, such that 𝑢_𝑛,𝑣_𝑛⇀(𝑢,𝑣)in𝑋₁,a.e.𝑡∈(0,∞). (3.16)
By (2.15), (2.16), and (2.17); and Rellich-Kondrachov Compactness Theorem, we know operator 𝛿𝐻𝑢₁,𝑢₂𝛿𝑢₂𝑢,−𝛿𝐻₁,𝑢₂𝛿𝑢₁∶𝑋₁→𝑋^∗₁ (3.17) is weakly continuous.
Let 𝑛→∞ in (3.8), following equality: (𝑢)+(𝑣)=𝑢,𝑣,_𝑡0𝛿𝐻(𝑢,𝑣),𝑢−()𝛿𝑣𝛿𝐻𝑢,𝑣,𝑣𝜙𝛿𝑢𝑑𝑡+₁,𝑢+𝜙₂,𝑣 (3.18) holds true for any 𝑢,𝑣∈⋃^∞_𝑛=1𝑋_𝑛.
Since ⋃^∞_𝑛=1𝑋_𝑛 is dense in 𝐻¹₀(Ω), equality (3.18) holds true for all (𝑢,𝑣)∈𝑋₁, which implies that (𝑢,𝑣)∈𝐿^∞((0,∞),𝑋₁) is a global solution of (3.3), then 𝜓=𝑢+𝑖𝑣∈𝐿^∞((0,∞),𝐻¹(Ω,𝐶)) is a global solution of (2.19).
At last, we prove the global solution 𝜓=𝑢+𝑖𝑣 of (2.19) is in 𝐶⁰([0,∞),𝐿²(Ω,𝐶)) by semigroup theory.
Set operator 𝐴∶=0−𝐿𝐿0. (3.19)
Since the following equality: 𝐴𝑢₁,𝑢₂,𝜔₁,𝜔₂=𝑢₁,𝑢₂,−𝐴𝜔₁,𝜔₂ (3.20) holds true for any (𝑢₁,𝑢₂),(𝜔₁,𝜔₂)∈𝑋₁, then operator 𝐴∶𝑋₁→𝑋^∗₁ is an antisymmetric operator. By Stone Theorem, operator 𝐴 is a generator of an unitary semigroup and the unitary semigroup can be represented as follows: 𝑇(𝑡)=cos𝑡𝐿−sin𝑡𝐿sin𝑡𝐿cos𝑡𝐿. (3.21)
The solution of (3.3) can be represented as follows: 𝑢=(cos𝑡𝐿)𝜓₁−(sin𝑡𝐿)𝜓₂+^𝑡₀[cos(𝑡−𝜏)𝐿]𝐺₁−[sin(𝑡−𝜏)𝐿]𝐺₂()𝜓𝑑𝜏,𝑣=sin𝑡𝐿₁+(cos𝑡𝐿)𝜓₂+^𝑡₀[sin(𝑡−𝜏)𝐿]𝐺₁+[cos(𝑡−𝜏)𝐿]𝐺₂𝑑𝜏, (3.22) where 𝐺₁=1ℏ𝑔^′𝑢²+𝑣²𝑢²+𝑣²1𝑣+ℏ𝑔𝑢²+𝑣²𝐺𝑣,₂1=−ℏ𝑔^′𝑢²+𝑣²𝑢²+𝑣²1𝑢−ℏ𝑔𝑢²+𝑣²𝑢. (3.23)
By (2.15), (2.16), and (2.17); and Gagliardo-Nirenberg-Sobolev inequality, we obtain that the global solution of (3.3) satisfies (𝑢,𝑣)∈𝐶⁰([0,∞),𝑋), which implies 𝜓=𝑢+𝑖𝑣∈𝐶⁰([0,∞),𝐿²(Ω,𝐶)).
Furthermore, the solution 𝜓 can be expressed as follows: 𝜓=(cos𝑡𝐿+𝑖sin𝑡𝐿)𝜓₀−𝑖ℎ^𝑡₀[cos(𝑡−𝜏)𝐿+𝑖sin(𝑡−𝜏)𝐿]𝐺𝜓𝑑𝜏. (3.24)

Remark 3.2. In [24], it was proved that all dynamic equations in quantum physics, that is, 𝑖ℏ𝜕𝜓_𝑘=𝜕𝑡𝛿𝐻𝛿𝜓^∗_𝑘,1≤𝑘≤𝑚, (3.25) can be equivalently expressed as the following Hamilton form: 𝜕𝜓¹_𝑘=𝜕𝑡𝛿𝐻𝛿𝜓²_𝑘,𝜕𝜓²_𝑘𝜕𝑡=−𝛿𝐻𝛿𝜓²_𝑘,(1≤𝑘≤𝑚), (3.26) where 𝐻 the Hamilton energy, 𝜓_𝑘 the wave function and 𝜓_𝑘=𝜓¹_𝑘+𝑖𝜓²_𝑘.

4. The Conservation Laws

For the NLS model (2.19), we prove that the Hamilton energy and the total particle number both are conservative quantities.

Theorem 4.1. Assume that 𝑔 satisfies conditions (2.15), (2.16) and (2.17), if 𝑉(𝑥)∈𝐿²(Ω), then for any 𝜓₀∈𝐻¹(Ω,𝐶), there exist two conservative quantities for (2.19): the energy 𝐻𝜓=_Ωℏ²4𝑚∇𝜓²+12𝑉(𝑥)𝜓²+12𝑔𝜓²𝜓²𝑑𝑥, (4.1) and the total particle number 𝑁=_Ω𝜓²𝑑𝑥. (4.2)

Proof. Since 𝜓=𝑢+𝑖𝑣 is the solution of (2.19), then (𝑢,𝑣) is the solution of (3.3) and we have the following equalities: 𝑑𝐻(𝑢,𝑣)=()𝑑𝑡𝛿𝐻𝑢,𝑣,𝛿𝑢𝜕𝑢+()𝜕𝑡𝛿𝐻𝑢,𝑣,𝛿𝑣𝜕𝑣()𝜕𝑡=−𝛿𝐻𝑢,𝑣,()𝛿𝑢𝛿𝐻𝑢,𝑣+()𝛿𝑣𝛿𝐻𝑢,𝑣,()𝛿𝑣𝛿𝐻𝑢,𝑣𝛿𝑢=0,𝑑𝑁𝑑𝑡=2_Ω𝑢𝜕𝑢𝜕𝑡+𝑣𝜕𝑣𝜕𝑡𝑑𝑥=2_Ω𝑢𝛿𝐻(𝑢,𝑣)()𝛿𝑣−𝑣𝛿𝐻𝑢,𝑣𝛿𝑢𝑑𝑥=2_Ω−ℏ12𝑚𝑢Δ𝑣+ℏ𝑉(𝑥)+1𝑢𝑣ℏ𝑔^′𝑢²+𝑣²𝑢²+𝑣²1𝑢𝑣+ℏ𝑔𝑢²+𝑣²𝑢𝑣𝑑𝑥−2_Ω−ℏ12𝑚𝑣Δ𝑢+ℏ𝑉(𝑥)+1𝑢𝑣ℏ𝑔^′𝑢²+𝑣²𝑢²+𝑣²1𝑢𝑣+ℏ𝑔𝑢²+𝑣²𝑢𝑣𝑑𝑥=2_Ω−ℏℏ2𝑚Δ𝑣𝑢+2𝑚Δ𝑢𝑣𝑑𝑥=2_Ωℏℏ2𝑚∇𝑢∇𝑣−2𝑚∇𝑣∇𝑢𝑑𝑥=0, (4.3) which imply that the energy 𝐻 and the total particle number 𝑁 both are conservative quantities of (2.19).

5. Discussion

Taking the dense fluid of strongly interacting bosons as mixture of normal fluid and superfluid, and substituting the rule of Galilean invariance for local gauge invariance, Coste [13] made correction for the Lagrangian of the original GP-model by adding the degrees of freedom corresponding to the normal fluid. As a result, they obtained the generalized GP-equation which can describe both the two-fluid model and the Hills-Roberts model under two different circumstances.

Building on the works of Gardiner [14] and Castin and Dum [15], Gardiner and Morgan [16] derived the generalized GP-equation which can describe the condensate and noncondensate dynamics of Bose-Einstein dilute atomic gas at finite temperature. It is worthwhile to mention that unlike using expansion in inverse powers of the total number of particles in [14], Gardiner and Morgan [16] used expansion in powers of ration of noncondensate to condensate particle numbers and constructed the approximate Hamiltonian of third-order.

As the same as the above works [13, 16], the manuscript presented here also derive the generalized GP-equation from the correction of the original Hamiltonian. In addition, collapse (blow up) is prevented for our model and also for condensate and noncondensate dynamic model [16] when accounting for fluctuations.

But differences do exist. One of the differences is that the two above works are based on the classification of the state of particle (or the state of fluid), that is, condensate and noncondensate (or normal fluid and superfluid), but ours focus on the classification of interaction of particles, that is, the s-wave scattering and the atom-atom interaction. And another difference is the mechanism on which above related models build. The two-fluid model [13] respect Galilean invariance rule. The condensate and noncondensate dynamic model [16] obey the formalism of number-conserving. However, our model builds on the basis of the wave-particle duality in quantum mechanics.

It must be pointed out that our model is valid only on three assumptions. One is that the interactions among particles include only two effects: the s-wave scattering and the atom-atom interaction. Consequently, there is no other effect. Another one is that atom-atom interaction be chosen to be the van der Waals force. And the third one is that the interaction potential energy is changed continuously with density of particles.

Meanwhile, it is that the global solution to the NLS model is well defined and collapse (blow-up) is prevented guaranteeing the model is reasonable from the mathematical viewpoint, but further physical experiments should be done to verify this model. Especially, data from future experiments combining with the conditions (2.15) and (2.16) may give the exact expression of function 𝑔.

Inspired by the classification of the state of particle (i.e., condensate and noncondensate) in works [9, 10, 15, 16], and taking into account of the classification of the interaction of particles (i.e., the s-wave scattering and the atom-atom interaction), further investigation on the model of general many-particle quantum systems is necessary in future.

6. Conclusions

Building on the basis of the wave-particle duality in quantum mechanics and assumption that the interactions among particles include only two effects: the s-wave scattering and the atom-atom interaction, we derive the new Hamilton energy from the correction of the original one. From the new Hamiltonian we derive the NLS model for more general many-particle quantum systems. Expression of the global solution to the NLS model is obtained. Collapse (blow-up) is prevented for the model. Conservation laws hold true both for the Hamilton energy and the total particle number.

Acknowledgments

The authors are grateful to the anonymous referees whose careful reading of the paper and valuable comments were very helpful for revising and improving our work, as well as for bringing references [9, 16] to our attention. This work is supported by the Scientific Research Foundation of Civil Aviation Flight University of China (J2011-30).