In the following discussion of the evolution of the density contrast, we assume that
Newtonian mechanics can be applied, an approximation which simplifies the study of the
development of structures significantly compared to Einstein's theory of gravity. This
assumption is well justified if we stay within the non-relativistic domain; i.e.
and (Hubble radius), where
is the size of the particle horizon and *H* is the Hubble parameter
at time *t*.

The matter will be treated as an ideal fluid, which will enable us to make use of the following three equations: the conservation of mass'

the Euler equation of motion,

and Poisson's equation for the gravitational potential ,

The velocity field and the mass density are both functions of
the physical coordinates and time *t*. The subscript in the equations
indicate that the term in question is to be calculated with respect to the proper
coordinates. But, as in equation (2.1), we would like to use comoving
coordinates. The relation between these two types of coordinates is as follows:

where *a*(*t*) is the scale factor describing the scale of the Universe as it
expands. The velocity field can then be written as

The first term on the right hand side is recognized as the Hubble flow, , and the last term is the peculiar velocity relative to the general expansion, . If we assume that and have small values; i.e. much less then unity, we can linearize equations (2.2)-(2.4). This assumption is well justified in the early epochs of the Universe and on large-scales, where the mass distribution is approximately homogeneous. If we combine the linearized version of equations (2.2)-(2.4), we get the time evolution equation of the mass density contrast in linear perturbation theory:

This equation is local; i.e. it is only dependent on the conditions at one point in space. It was this equation Lif deduced.

Let us now take a look at some solutions of equation (2.7), assuming
, where *p* is pressure and is the cosmological constant. The
easiest solution is for the Einstein-de Sitter model, where there is no space curvature
(*k*=0). The Friedmann-equations then gives us the following time evolution of the scale
parameter *a*:

If we insert this relation into equation (2.7), we get

a partial differential equation which has the solution

where *A* and *B* are constants. Based on this solution, Lif jumped
to the conclusion that the gravitational instability theory could not be used to explain
the formation of structures in the Universe; the growth would be too slow compared with
the exponential growth in a non-expanding Universe, which was the leading model at the
time.

Another solution when can be found by rewriting the Friedmann-equations as

where is the density parameter and *z* is the cosmological redshift
give by (subscript ``0'' denotes the present value). At large redshifts;
i.e. , we get the Einstein-deSitter model, and equation
(2.10) is valid for all models. If we have
an open model, and equation (2.11) will reduce to the Milne-model, where
and . If we insert this into equation (2.7)
we get

which has the solution

These two solutions in equation (2.10) and (2.13) tell us that the perturbations will, assuming a model, initially grow , but later, after , grow slower and finally end up with a constant amplitude.

So far we have ignored any pressure in the fluid, which at early epochs of the Universe
is a bad assumption. If we introduce pressure, the time evolution equation or the mass
density contrast will be coordinate dependent, which was not the case for *p*=0. If we
simplify the picture by assuming an ideal gas, we can, with help of equation
(2.1), deduce , where is the
speed of sound. This brings the density perturbation equation (2.7) to

To see the effect of the pressure term, we can write the density contrast as a Fourier series,

where the proper wavelength is . The coefficients in equation (2.15) is independent of , which gives us the following equation for each number vector:

The source terms on the right-hand side vanishes at wavelength

which is often referred to as the Jeans length. This was the scale Jeans-02 deduced as being the maximum size a gas cloud could have without collapsing. What does equation (2.16) tell us? Let's take a look at two special cases: If ; i.e. the wavelengths are long compared to the Jeans length, the pressure term in equation (2.14) becomes negligible, and we can apply the zero pressure solution. At wavelengths shorter then , the density contrast oscillates as a sound wave, which means that a density perturbations can not grow if it's scale is less then the Jeans length. If we have perturbations with amplitude decreasing with scale, the ones with will be the first to become non-linear.

Mon Jul 5 02:59:28 MET DST 1999