This articleneeds additional citations forverification. Please helpimprove this article byadding citations to reliable sources. Unsourced material may be challenged and removed. Find sources: "Ideal chain" – news ·newspapers ·books ·scholar ·JSTOR(April 2025) (Learn how and when to remove this message)

Anideal chain (orfreely-jointed chain) is the simplestmodel inpolymer chemistry to describepolymers, such asnucleic acids andproteins. It assumes that themonomers in a polymer are located at the steps of a hypotheticalrandom walker that does not remember its previous steps. By neglecting interactions amongmonomers, this model assumes that two (or more) monomers can occupy the same location. Although it is simple, its generality gives insight about thephysics of polymers.

In this model, monomers are rigid rods of a fixed lengthl, and their orientation is completely independent of the orientations and positions of neighbouring monomers. In some cases, the monomer has a physical interpretation, such as anamino acid in apolypeptide. In other cases, a monomer is simply a segment of the polymer that can be modeled as behaving as a discrete, freely jointed unit. If so,l is theKuhn length. For example,chromatin is modeled as a polymer in which each monomer is a segment approximately14–46 kbp in length.^[1]

Nmers form the polymer, whose total unfolded length is:$${\displaystyle L=Nl,}$$ whereN is the number of mers.

In this very simple approach where no interactions between mers are considered, the energy of the polymer is taken to be independent of its shape, which means that atthermodynamic equilibrium, all of its shape configurations are equally likely to occur as the polymer fluctuates in time, according to theMaxwell–Boltzmann distribution.

Let us call${\displaystyle \overrightarrow{R}}$ the total end to end vector of an ideal chain and${\displaystyle {\overrightarrow{r}}_1,\dots ,{\overrightarrow{r}}_N}$ the vectors corresponding to individual mers. Those random vectors have components in the three directions of space. Most of the expressions given in this article assume that the number of mersN is large, so that thecentral limit theorem applies. The figure below shows a sketch of a (short) ideal chain.

The two ends of the chain are not coincident, but they fluctuate around each other, so that of course:$${\displaystyle ⟨\overrightarrow{R}⟩=\sum _{i=1}^N⟨{\overrightarrow{r}}_i⟩=\overrightarrow{0}}$$

Throughout the article the${\displaystyle ⟨⟩}$ brackets will be used to denote themean (of values taken over time) of a random variable or a random vector, as above.

Since${\displaystyle {\overrightarrow{r}}_1,\dots ,{\overrightarrow{r}}_N}$ areindependent, it follows from thecentral limit theorem that${\displaystyle \overrightarrow{R}}$ is distributed according to anormal distribution (or gaussian distribution): precisely, in 3D,${\displaystyle R_x,R_y,}$ and${\displaystyle R_z}$ are distributed according to anormal distribution ofmean 0 and ofvariance:$${\displaystyle {\sigma }^2=⟨R_x^2⟩-⟨R_x{⟩}^2=⟨R_x^2⟩-0}$$$${\displaystyle ⟨R_x^2⟩=⟨R_y^2⟩=⟨R_z^2⟩=N\frac{l^2}{3}}$$

So that${\displaystyle ⟨R^2⟩=N{l}^2=Ll}$. The end to end vector of the chain is distributed according to the followingprobability density function:$${\displaystyle P(\overrightarrow{R})={\left(\frac{3}{2\pi N{l}^2}\right)}^{3/2}{e}^{-\frac{3{\left|\overrightarrow{R}\right|}^2}{2N{l}^2}}}$$

The average end-to-end distance of the polymer is:$${\displaystyle \sqrt{⟨R^2⟩}=\sqrt{N}l=\sqrt{Ll}}$$

A quantity frequently used in polymer physics is theradius of gyration:$${\displaystyle ⟨{\mathit{R}}_G⟩=\frac{\sqrt{N}l}{\sqrt{6}}}$$

It is worth noting that the above average end-to-end distance, which in the case of this simple model is also the typical amplitude of the system's fluctuations, becomes negligible compared to the total unfolded length of the polymer${\displaystyle Nl}$ at thethermodynamic limit. This result is a general property of statistical systems.

Mathematical remark: the rigorous demonstration of the expression of the density of probability${\displaystyle P(\overrightarrow{R})}$ is not as direct as it appears above: from the application of the usual (1D)central limit theorem one can deduce that${\displaystyle R_x}$,${\displaystyle R_y}$ and${\displaystyle R_z}$ are distributed according to a centerednormal distribution of variance${\displaystyle N{l}^2/3}$. Then, the expression given above for${\displaystyle P(\overrightarrow{R})}$ is not the only one that is compatible with such distribution for${\displaystyle R_x}$,${\displaystyle R_y}$ and${\displaystyle R_z}$. However, since the components of the vectors${\displaystyle {\overrightarrow{r}}_1,\dots ,{\overrightarrow{r}}_N}$ areuncorrelated for the random walk we are considering, it follows that${\displaystyle R_x}$,${\displaystyle R_y}$ and${\displaystyle R_z}$ are alsouncorrelated. This additional condition can only be fulfilled if${\displaystyle \overrightarrow{R}}$ is distributed according to${\displaystyle P(\overrightarrow{R})}$. Alternatively, this result can also be demonstrated by applying a multidimensional generalization of thecentral limit theorem, or throughsymmetry arguments.

While the elementary model described above is totally unadapted to the description of real-world polymers at the microscopic scale, it does show some relevance at the macroscopic scale in the case of a polymer in solution whose monomers form an ideal mix with the solvent (in which case, the interactions between monomer and monomer, solvent molecule and solvent molecule, and between monomer and solvent are identical, and the system's energy can be considered constant, validating the hypotheses of the model).

The relevancy of the model is, however, limited, even at the macroscopic scale, by the fact that it does not consider any excluded volume for monomers (or, to speak in chemical terms, that it neglectssteric effects). Since theN mers are of a rigid, fixed length, the model also does not consider bond stretching, though it can be extended to do so.^[2]

Other fluctuating polymer models that consider no interaction between monomers and no excluded volume, like theworm-like chain model, are all asymptotically convergent toward this model at thethermodynamic limit. For purpose of this analogy aKuhn segment is introduced, corresponding to the equivalent monomer length to be considered in the analogous ideal chain. The number of Kuhn segments to be considered in the analogous ideal chain is equal to the total unfolded length of the polymer divided by the length of a Kuhn segment.

If the two free ends of an ideal chain are pulled apart by some sort of device, then the device experiences a force exerted by the polymer. As the ideal chain is stretched, its energy remains constant, and its time-average, orinternal energy, also remains constant, which means that this force necessarily stems from a purelyentropic effect.

Thisentropic force is very similar to the pressure experienced by the walls of a box containing anideal gas. Theinternal energy of anideal gas depends only on its temperature, and not on the volume of its containing box, so it is not anenergy effect that tends to increase the volume of the box like gaspressure does. This implies that thepressure of an ideal gas has a purelyentropic origin.

What is the microscopic origin of such anentropic force or pressure? The most general answer is that the effect of thermal fluctuations tends to bring athermodynamic system toward a macroscopic state that corresponds to a maximum in the number of microscopic states (or micro-states) that are compatible with this macroscopic state. In other words, thermal fluctuations tend to bring a system toward its macroscopic state of maximumentropy.

What does this mean in the case of the ideal chain? First, for our ideal chain, a microscopic state is characterized by the superposition of the states${\displaystyle {\overrightarrow{r}}_i}$ of each individual monomer (withi varying from1 toN). In its solvent, the ideal chain is constantly subject to shocks from moving solvent molecules, and each of these shocks sends the system from its current microscopic state to another, very similar microscopic state. For an ideal polymer, as will be shown below, there are more microscopic states compatible with a short end-to-end distance than there are microscopic states compatible with a large end-to-end distance. Thus, for an ideal chain, maximizing itsentropy means reducing the distance between its two free ends. Consequently, a force that tends to collapse the chain is exerted by the ideal chain between its two free ends.

In this section, themean of this force will be derived. The generality of the expression obtained at thethermodynamic limit will then be discussed.

The case of an ideal chain whose two ends are attached to fixed points will be considered in this sub-section. The vector${\displaystyle \overrightarrow{R}}$ joining these two points characterizes the macroscopic state (or macro-state) of the ideal chain. Each macro-state corresponds a certain number of micro-states, that we will call${\displaystyle \mathrm{\Omega }(\overrightarrow{R})}$ (micro-states are defined in the introduction to this section). Since the ideal chain'senergy is constant, each of these micro-states is equally likely to occur. Theentropy associated to a macro-state is thus equal to:$${\displaystyle S(\overrightarrow{R})=k_{\text{B}}\log (\mathrm{\Omega }(\overrightarrow{R})),}$$where${\displaystyle k_{\text{B}}}$ is theBoltzmann constant

The above expression gives the absolute (quantum)entropy of the system. A precise determination of${\displaystyle \mathrm{\Omega }(\overrightarrow{R})}$ would require a quantum model for the ideal chain, which is beyond the scope of this article. However, we have already calculated the probability density${\displaystyle P(\overrightarrow{R})}$ associated with theend-to-end vector of theunconstrained ideal chain, above. Since all micro-states of the ideal chain are equally likely to occur,${\displaystyle P(\overrightarrow{R})}$ is proportional to${\displaystyle \mathrm{\Omega }(\overrightarrow{R})}$. This leads to the following expression for the classical (relative)entropy of the ideal chain:$${\displaystyle S(\overrightarrow{R})=k_{\text{B}}\log (P(\overrightarrow{R}))+C_{st},}$$where${\displaystyle C_{st}}$ is a fixed constant. Let us call${\displaystyle \overrightarrow{F}}$ the force exerted by the chain on the point to which its end is attached. From the above expression of theentropy, we can deduce an expression of this force. Suppose that, instead of being fixed, the positions of the two ends of the ideal chain are now controlled by an operator. The operator controls the evolution of the end to end vector${\displaystyle \overrightarrow{R}}$. If the operator changes${\displaystyle \overrightarrow{R}}$ by a tiny amount${\displaystyle d\overrightarrow{R}}$, then the variation ofinternal energy of the chain is zero, since theenergy of the chain is constant. This condition can be written as:$${\displaystyle 0=dU=\delta W+\delta Q}$$

${\displaystyle \delta W}$ is defined as the elementary amount ofmechanical work transferred by the operator to the ideal chain, and${\displaystyle \delta Q}$ is defined as the elementary amount of heat transferred by the solvent to the ideal chain. Now, if we assume that the transformation imposed by the operator on the system is quasistatic (i.e., infinitely slow), then the system's transformation will be time-reversible, and we can assume that during its passage from macro-state${\displaystyle \overrightarrow{R}}$ to macro-state${\displaystyle \overrightarrow{R}+d\overrightarrow{R}}$, the system passes through a series ofthermodynamic equilibrium macro-states. This has two consequences:

1. first, the amount ofheat received by the system during the transformation can be tied to the variation of itsentropy:$${\displaystyle \delta Q=TdS,}$$ whereT is the temperature of the chain.
2. second, in order for the transformation to remain infinitely slow, themean force exerted by the operator on the end points of the chain must balance themean force exerted by the chain on its end points. Calling${\displaystyle {\overrightarrow{f}}_{\text{op}}}$ the force exerted by the operator and${\displaystyle \overrightarrow{f}}$ the force exerted by the chain, we have:$${\displaystyle \delta W=⟨{\overrightarrow{f}}_{\text{op}}⟩\cdot d\overrightarrow{R}=-⟨\overrightarrow{f}⟩\cdot d\overrightarrow{R}}$$

We are thus led to:$${\displaystyle ⟨\overrightarrow{f}⟩=T\frac{dS}{d\overrightarrow{R}}=\frac{k_{\text{B}}T}{P(\overrightarrow{R})}\frac{dP(\overrightarrow{R})}{d\overrightarrow{R}}}$$$${\displaystyle ⟨\overrightarrow{f}⟩=-k_{\text{B}}T\frac{3\overrightarrow{R}}{N{l}^2}}$$

The above equation is theequation of state of the ideal chain. Since the expression depends on thecentral limit theorem, it is only exact in the limit of polymers containing a large number of monomers (that is, thethermodynamic limit). It is also only valid for small end-to-end distances, relative to the overall polymercontour length, where the behavior is like a hookean spring. Behavior over larger force ranges can be modeled using acanonical ensemble treatment identical to magnetization of paramagnetic spins. For the arbitrary forces the extension-force dependence will be given byLangevin function${\displaystyle \mathcal{L}}$:$${\displaystyle \frac{R}{Nl}=\coth \left(\frac{fl}{k_{\text{B}}T}\right)-\frac{k_{\text{B}}T}{fl}=\mathcal{L}\left(\frac{fl}{k_{\text{B}}T}\right),}$$where the extension is${\displaystyle R=|\overrightarrow{R}|}$.

For the arbitrary extensions the force-extension dependence can be approximated by:^[3]$${\displaystyle \frac{fl}{k_{\text{B}}T}={\mathcal{L}}^{-1}\left(\frac{R}{Nl}\right)\approx 3\frac{R}{Nl}+\frac{1}{5}{\left(\frac{R}{Nl}\right)}^2\sin \left(\frac{7R}{2Nl}\right)+\frac{{\left(\frac{R}{Nl}\right)}^3}{1-\frac{R}{Nl}},}$$where${\displaystyle {\mathcal{L}}^{-1}}$ is the inverseLangevin function,N is the number of bonds^[4] in the molecule (therefore if the molecule hasN bonds it hasN + 1 monomers making up the molecule.).

Finally, the model can be extended to even larger force ranges by inclusion of a stretch modulus along the polymer contour length. That is, by allowing the length of each unit of the chain to respond elastically to the applied force.^[5]

Throughout this sub-section, as in the previous one, the two ends of the polymer are attached to a micro-manipulation device. This time, however, the device does not maintain the two ends of the ideal chain in a fixed position, but rather it maintains a constant pulling force${\displaystyle {\overrightarrow{f}}_{\text{op}}}$ on the ideal chain. In this case the two ends of the polymer fluctuate around amean position${\displaystyle ⟨\overrightarrow{R}⟩}$. The ideal chain reacts with a constant opposite force${\displaystyle \overrightarrow{f}=-{\overrightarrow{f}}_{\text{op}}}$.

For an ideal chain exchanging length with a reservoir, a macro-state of the system is characterized by the vector${\displaystyle \overrightarrow{f}}$.

The change between an ideal chain of fixed length and an ideal chain in contact with a length reservoir is very much akin to the change between the micro-canonical ensemble and the canonical ensemble (see theStatistical mechanics article about this).^[6] The change is from a state where a fixed value is imposed on a certain parameter, to a state where the system is left free to exchange this parameter with the outside. The parameter in question is energy for the microcanonical and canonical descriptions, whereas in the case of the ideal chain the parameter is the length of the ideal chain.

As in the micro-canonical and canonical ensembles, the two descriptions of the ideal chain differ only in the way they treat the system's fluctuations. They are thus equivalent at thethermodynamic limit. Theequation of state of the ideal chain remains the same, except that${\displaystyle \overrightarrow{R}}$ is now subject to fluctuations:$${\displaystyle \overrightarrow{f}=-k_{\text{B}}T\frac{3⟨\overrightarrow{R}⟩}{N{l}^2}.}$$

Consider a freely jointed chain of${\displaystyle N}$ bonds of length${\displaystyle l}$ subject to a constant elongational force${\displaystyle f}$ applied to its ends along the${\displaystyle z}$ axis and an environment temperature${\displaystyle T}$. An example could be a chain with two opposite charges${\displaystyle +q}$ and${\displaystyle -q}$ at its ends in a constantelectric field${\displaystyle \overrightarrow{E}}$ applied along the${\displaystyle z}$ axis as sketched in the figure on the right. If the directCoulomb interaction between the charges is ignored, then there is a constant force${\displaystyle \overrightarrow{f}}$ at the two ends.

Different chain conformations are not equally likely, because they correspond to different energy of the chain in the external electric field.$${\displaystyle U=-q\overrightarrow{E}\cdot \overrightarrow{R}=-\overrightarrow{f}\cdot \overrightarrow{R}=-f{R}_z}$$

Thus, different chain conformation have different statisticalBoltzmann factors${\displaystyle \exp (-U/k_{\text{B}}T)}$.^[4]

Thepartition function is:$${\displaystyle Z=\sum _{\text{states}}\exp (-U/k_{\text{B}}T)=\sum _{\text{states}}\exp \left(\frac{f{R}_z}{k_{\text{B}}T}\right)}$$

Everymonomer connection in the chain is characterized by a vector${\displaystyle {\overrightarrow{r}}_i}$ of length${\displaystyle l}$ and angles${\displaystyle {\theta }_i,{\phi }_i}$ in thespherical coordinate system. The end-to-end vector can be represented as:$R_z=\sum _{i=1}^{N}l\cos {\theta }_i$. Therefore:

TheGibbs free energy G can be directly calculated from the partition function:$${\displaystyle G(T,f,N)=-k_{\text{B}}T\ln Z(T,f,N)=-N{k}_{\text{B}}T\left[\ln \left(4\pi \sinh \left(\frac{fl}{k_{\text{B}}T}\right)\right)-\ln \left(\frac{fl}{k_{\text{B}}T}\right)\right]}$$

The Gibbs free energy is used here because the ensemble of chains corresponds to constant temperature${\displaystyle T}$ and constant force${\displaystyle f}$ (analogous to theisothermal–isobaric ensemble, which has constant temperature and pressure).

The average end-to-end distance corresponding to a given force can be obtained as the derivative of the free energy:$${\displaystyle ⟨R⟩=-\frac{\mathrm{\partial }G}{\mathrm{\partial }f}=Nl\left[\coth \left(\frac{fl}{k_{\text{B}}T}\right)-\frac{k_{\text{B}}T}{fl}\right]}$$

This expression is theLangevin function${\displaystyle \mathcal{L}}$, also mentioned in previous paragraphs:

$${\displaystyle \mathcal{L}(\alpha )=\coth (\alpha )-\frac{1}{\alpha }}$$where${\displaystyle \alpha =\frac{fl}{k_{\text{B}}T}}$.

For small relative elongations (${\displaystyle ⟨R⟩\ll R_{\text{max}}=lN}$) the dependence is approximately linear,$${\displaystyle \mathcal{L}(\alpha )\cong \frac{\alpha }{3}\text{ for }\alpha \ll 1}$$and followsHooke's law as shown in previous paragraphs:$${\displaystyle \overrightarrow{f}=k_{\text{B}}T\frac{3⟨\overrightarrow{R}⟩}{N{l}^2}}$$

• Polymer
• Worm-like chain, a more complex polymer model
• Kuhn length
• Coil–globule transition

• Polymer chemistry
• Polymer physics

• Articles with short description
• Short description is different from Wikidata
• Articles needing additional references from April 2025
• All articles needing additional references