One measure of the voltage dependence of ion channel conductance is the amount of gating charge that moves during activation and vice versa. The limiting slope method, introduced by Almers (Almers, W. 1978. *Rev. Physiol. Biochem. Pharmacol.* 82:96–190), exploits the relationship of charge movement and voltage sensitivity, yielding a lower limit to the range of single channel gating charge displacement. In practice, the technique is plagued by low experimental resolution due to the requirement that the logarithmic voltage sensitivity of activation be measured at very low probabilities of opening. In addition, the linear sequential models to which the original theory was restricted needed to be expanded to accommodate the complexity of mechanisms available for the activation of channels. In this communication, we refine the theory by developing a relationship between the mean activation charge displacement (a measure of the voltage sensitivity of activation) and the gating charge displacement (the integral of gating current). We demonstrate that recording the equilibrium gating charge displacement as an adjunct to the limiting slope technique greatly improves accuracy under conditions where the plots of mean activation charge displacement and gross gating charge displacement versus voltage can be superimposed. We explore this relationship for a wide variety of channel models, which include those having a continuous density of states, nonsequential activation pathways, and subconductance states. We introduce new criteria for the appropriate use of the limiting slope procedure and provide a practical example of the theory applied to low resolution simulation data.

## Introduction

The sine qua non of voltage-dependent ion channels is their ability to alter ion permeability of membranes in response to changes in the transmembrane potential. Hodgkin and Huxley (1952) accounted for the voltage sensitivity of Na^{+} and K^{+} conductance in the squid giant axon by postulating charge movement between kinetically distinct states of hypothetical “activating particles”. With the advances that have been made in the biochemistry and molecular biology of ion channels since then, we now recognize that the embodiment of their “activating particle” resides in the ion channel itself, as a structural component, though the molecular details of the voltage sensitive “gating” of the pore remains largely unknown. The first verification of gating charge movement was by Armstrong and Bezanilla (1973), who recorded nonlinear capacitive current transients from tetrodotoxin (TTX) blocked Na channels in the squid axon. An important quantity that characterizes the voltage sensitivity of the channel is the range of gating charge displacement Δ*q* energetically linked to channel activation. The most significant advancement in measuring Δ*q* that followed the work of Hodgkin and Huxley was due to Almers (1978), who treated the case of a linear sequence of discrete closed states followed by a single open state (Almers' criterion, see Fig. 1 *A*). Almers stated that for such a model, the following relation holds:

where *P*_{o} is the fraction of time the channel is open at equilibrium (open probability), *V* is the membrane potential in millivolts, and *kT* is the characteristic thermal energy (Boltzmann constant times absolute temperature ≃ 25 milli-electron volts at room temperature). The experimental use of Eq. 1, often referred to as the limiting slope procedure, has been used by many investigators to estimate total gating charge movement of activation (e.g., Stimers et al., 1985; Liman et al., 1991; Papazian et al., 1991; Schoppa et al., 1992; Zagotta et al., 1994).

The *Q*/*N* technique is an alternative to the limiting slope method and is a direct determination of gating charge movement per channel. Independent measurements of the total charge *Q* and the number of channels *N* are made in a single preparation, and the ratio, Δ*q*_{Q/N}, is then calculated. The first reliable value of Δ*q*_{Q/N} was published by Schoppa et al. (1992), who recorded from a single patch containing *Shaker* K^{+} channels expressed in *Xenopus* oocytes. They obtained a Δ*q*_{Q/N} of 12.3 eu (electronic unit of charge ≃ 1.602 × 10^{−19} Coulumbs)^{1} per channel, which has since been verified by our lab and others (Aggarwal and MacKinnon, 1996; Noceti et al., 1996; Seoh et al., 1996). A similar value was obtained from a mutant channel in which the hydrophobic residue Leu^{370}, located in the putative voltage sensing domain of *Shaker* (the S4 transmembrane segment), was replaced with valine. Their finding of no change in Δ*q*_{Q/N} in the mutant compared to the unmutated channel was expected since the net charge of the protein was unchanged. However, use of the limiting slope procedure on the two channels yielded values that were significantly lower than Δ*q*_{Q/N}: 9.5 eu for the unmutated channel and 5.5 eu for the mutant (Schoppa et al., 1992). The discrepancy between the results from the *Q*/*N* technique and the limiting slope procedure might be explained by the existence of gating charge movement which is dissociated from the activation process, making no contribution to voltage sensitivity of opening. This noncontributing charge component may take on two forms: gating charge movement occurring after the channel has opened (latent charge movement) and charge movement that is independent of the activation process (peripheral charge movement). The limiting slope procedure, in contrast to the *Q*/*N* technique, measures only the range of charge movement which is energetically linked to channel opening (activation charge movement), ignoring the latent and peripheral charge movements. In their conclusion, Schoppa et al. were careful to point out that, despite the possibility that latent and/or peripheral charge movement exists in *Shaker,* the most likely source for the reduced limiting slope values was lack of experimental resolution. Indeed, there has been sharp criticism of the reliability of the limiting slope procedure from various authors (Anderson and Koeppe, 1992; Bezanilla and Stefani, 1994; Zagotta et al., 1994). The chief reasons for the skepticism in the validity of the technique are: (*a*) the inability to accurately determine where the limiting value of the slope occurs on the voltage axis and (*b*) the difficulty of measuring the low values *P*_{o} required to reach that value (typically <10^{−3}).

In this paper, we address the problem of poor resolution in the limiting slope procedure by introducing a measure of the progress of activation named the activation charge displacement, *q*_{a}. Plotting mean activation charge displacement 〈*q*_{a}〉 versus voltage is a more reliable way of estimating limiting slope, and, furthermore, there is a relation between 〈*q*_{a}〉 and mean gating charge displacement, 〈*q*〉, which makes the additional measurement of gating currents a valuable tool in interpreting limiting slope data (for example, the gating current recordings by Schoppa et al. (1992) can be used to predict the amount by which they underestimated Δ*q* with the limiting slope technique). We develop the theory to include models containing an arbitrary number and arrangement of states (including continuum models) and allow for multiple open states with different conductances. We follow with a series of examples illustrating the theory, ending with a sample analysis of low resolution simulated data. We conclude with a summary of results and an approach for applying the limiting slope method in practice.

### Theory

#### Nature of the model.

We preface the discussion of specific models by stating assumptions regarding their general nature. We assume that after a sudden step in membrane potential, the occupancy distribution of the channel propagates through a network of conformational states representing the activation pathway. The reaction coordinate is the gating charge displacement (*q*). To place the quantity *q* in its proper context, we note that the mean gating current for *N* channels 〈*I*_{g}〉 is *N*d〈*q*〉*/*d*t* and the plot of *N*〈*q*〉 vs. voltage is the *Q* -*V* curve. There may be more than one state for a given value of *q*, which allows for loops and parallel pathways in the activation sequence (see Fig. 1,*B*). Since the mean 〈*q*〉 is an extensive state variable, *q* has a specific value for every state in the model. In addition, states are assigned a potential of mean force *F(q,*ξ*,V)* and a fractional conductance *f(q,*ξ*)*. Both are assumed to be defined by the value of *q* and other degrees of freedom indicated by ξ, and, in the case of *F*, also the membrane potential *V*. In terms of the variable ξ, we will be pri-marily concerned with degrees of freedom produced by states that are degenerate with respect to *q*. An example is a branching of the activation path, producing a duplication of states. Accordingly, in some cases it is useful to include a degeneracy factor φ, which for a nondegenerate state has the value of one. We assume for the purpose of derivations that all gating charge is energetically coupled to the activation process (essential charge), since only essential charge contributes to the voltage sensitivity of activation. We shall consider the effect of peripheral charge in Fig. 4. The fractional conductance is defined as the ratio of the state conductance *g*(*q*) to the maximal value at the given potential, *g*_{o}. We assume a linear voltage-dependence of *F*(*q*,*V*) (e.g., Tsien and Noble, 1969):

where *G*(*q*) = *F*(*q*,*0*) and depends on thermodynamic variables other than voltage such as temperature and pressure. By assigning a set of variables to each state rather than a difference of values between states (as is often done in describing kinetic models), we assure that the model automatically obeys detailed balance and conservation of charge density around any loops in the kinetic model. In this paper we consider only thermodynamic quantities, so we ignore the nature of pathways between states that determine kinetics. We require only that equilibration occurs between states on a time scale which is faster than that of our method of measurement (see Fig. 9 and corresponding text).

#### Definition of terms.

The word activation refers to the process of opening the channel pore. Technically, then, a blocked channel does not activate, but in such cases we alter the definition to include any conformational changes in the channel protein that produces a change in gating charge displacement. Without loss in generality, we assume that conducting channels activate with increasing membrane potential, since most classes of ion channels conform to this behavior. However, the theory outlined below is easily applied to a channel that opens with hyperpolarization by making trivial changes in sign. We formally define gating charge displacement *q* as any nonlinear capacitive charge movement in a single channel, regardless of whether it makes an energetic contribution to opening (activation coupling) or not. The variable *q* serves as a convenient reaction coordinate of activation. The value of *q* in the limit *V* → −Θ is referenced to zero. The maximum value of *q* at depolarizing potentials is by definition the total gating charge movement per channel Δ*q*, which is measurable experimentally with the *Q*/*N* procedure, i.e. Δ*q* = Δ*q*_{Q/N}. The component of *q* which is activation coupled is the essential charge displacement (*q*_{e}) and the remainder is the peripheral charge displacement (*q*_{p}). The latter does not contribute to the voltage sensitivity of the channel. The open probability (*P*_{o}) is defined for a population of channels as the ratio of the mean conductance to the maximum conductance. We introduce the activation potential (*W*_{a} = *−kT* ln[*P*_{o}]), which is a measure of the electrical energy needed to open the channel. Finally, we define the activation charge displacement (*q*_{a}) through its mean value, which equals the negative gradient of the activation potential: 〈*q*_{a}〉 = *−*d*W*_{a}*/*d*V*. Note that if *P*_{o} is multiplied by a constant it does not affect the value of 〈*q*_{a}〉, i.e.,

This is useful experimentally since the value of *P*_{o} obtained from analysis of macroscopic ionic current traces is usually defined only within a multiplicative constant. In the next two sections we will derive a relationship between the mean activation charge and gating charge displacements that will serve as the foundation for developing a practical approach in measuring essential gating charge movement.

#### Finite number of states.

We start with models that contain a finite number of discrete states, by which we mean that the time spent by the channel during the transition from one state to another is negligible compared to the dwell times in the states themselves. For the purpose of this derivation, and the one following which deals with continuum models, all gating charge movement is essential (i.e., *q* = *q*_{e}). Each state *i* is completely specified by the state variables (*q*_{i}, *G*_{i}, *f*_{i}) as well as an optional degeneracy factor φ_{i}. Subconductance states are produced when 0 < *f*_{i} < 1. The open probability of a single channel at equilibrium is *P*_{o} = 〈*g*〉/*g*_{o}, where *g*_{o} is the open pore conductance, and 〈*g*〉 is the average conductance.

The *p*_{i} are the equilibrium state probabilities which are found using the normalized Boltzmann distribution:

The denominator in Eq. 5 has the form of a coarse-grained partition function. From Eqs. 4 and 5 we obtain an expression for the mean open probability:

Then, using the linear relation of Eq. 2, which for a discrete model has the form:

The two terms on the right side of Eq. 8 are averages over *q*. The first term uses a reduced partition function where each term is weighted by the fractional conductance of the corresponding state. The second term, which sums over all states, is the average gating charge displacement 〈*q*〉, which, in the absence of peripheral charge movement, is proportional to the experimentally derived *Q*-*V* curve. We rewrite Eq. 8 as:

The second term on the right of Eq. 9, which sums over states that have at least partial conductance, represents the mean latent charge displacement (〈*q*_{l}〉). In the expression for 〈*q*_{l}〉, the quantity that is being averaged over is Δ*q* − *q*, which has its origin where the gating charge displacement reaches its largest value (i.e., *q* = Δ*q*) and increases with decreasing value of *q*. Thus, for example, the open state in the model of Fig. 1 *A*, although it conducts (f ≠ 0), contributes nothing towards the value of 〈*q*_{l}〉 because it lies to the right of all the other states, at the value of maximum gating charge displacement.

Finally, after moving 〈*q*_{l}〉 to the left side of the equation, we have:

The relationship between the activation and essential charge displacements is now clear. The sum of the activation and latent charge displacement curves (〈*q*_{a}〉 + 〈*q*_{l}〉) superimposes onto that of the mean gating charge displacement 〈*q*〉 by simply inverting and shifting upwards by Δ*q*. In the event that 〈*q*_{l}〉 vanishes or remains constant for all potentials, 〈*q*_{a}〉 can be superimposed onto 〈*q*〉. In such cases, we say that the channel is saturated with activation charge, since the total range of activation charge displacement (Δ*q*_{a}) matches the charge movement per channel, Δ*q*. In a saturated channel, knowledge of the shape of 〈*q*〉 versus voltage, obtainable from a *Q-V* measurement, allows one to predict the range in potentials where 〈*q*_{a}〉 reaches its limiting value. A model that satisfies Almers' criterion (Fig. 1 *A*) is obviously saturated. However, so are kinetic models with a more complicated arrangement (loops and parallel pathways) of closed states that converge onto a single or degenerate set of open state(s). The requirement for saturation is twofold: (*a*) the activation sequence has only one open state, or, if there is a cluster of open states, they must all have the same value of *q* ; (*b*) there is no peripheral charge movement. If the first requirement is satisfied, but not the second, then we can speak of saturation of the essential activation sequence. However, the presence of peripheral charge movement may contaminate the shape of the *Q* -*V*, making it less useful for limiting slope analysis. In any case, Eq. (10) can be made generally valid even when there is peripheral charge movement by replacing *q* with *q*_{e}.

#### Continuous density of states.

A similar analysis can be applied to a continuous system. Here, the partition function becomes an integral over a continuum of states. We maintain the condition that the only variable to be summed over is the gating charge *q*. The meaning of *f*(*q*) in a continuum model may be best thought of as a conditional probability relating *q* to the likelihood that the pore is open. With these considerations in mind, the derivation follows exactly that of the discrete state model. The continuum analogue of Eq. 6 is:

As we did in the case of discrete models, we identify the second term on the right of Eq. 12 as the latent charge position 〈*q*_{l}〉. Obviously, 〈*q*_{l}〉 cannot be made to vanish or even maintain a constant value with respect to voltage without rendering the channel permanently closed. This is because, in order for the channel to conduct at all, *f*(*q*) must have a nonvanishing value across some range of the continuous variable *q*. In other words, it is meaningless to speak of a single open state in a continuum model, and so the channel will never be saturated with activation charge. However, one can come close (within experimental resolution) by allowing the channel to be open only for a range of values of *q* near its maximum value (e.g., see Fig. 7).

## Methods

### Numerical Computation of Activation Curves

Activation curves of discrete state models were calculated using Eqs. 5–7, 9, and 10 from the array of state variables (*q*_{i}, *G*_{i}, *f*_{i}) and degeneracy factors φ_{i} that define a particular model. Continuum models were evaluated using the same algorithm by increasing the number of “states” to 2,000. It was found that as few as 50 states were needed for the numerical solution to converge within 3% of the continuum solution.

### Ramp Simulations

Simulation of ramp experiments were performed with a Monte Carlo algorithm. The long period (>2 × 10^{18}) random number generator of L'Ecuyer with Bays-Durham shuffle (Press et al., 1992) was used to generate random numbers *r*_{n} with values between 0 and 1. Waiting times τ_{ab} of transitions from state *a* to state *b* were calculated from transformation of *r*_{n}. Unlike the situation where the membrane potential is held constant over the time course of simulation, the distribution of waiting times for an applied voltage ramp is not exponential since the value of the unidirectional rate constant α_{ab} changes with time. According to the theory of failure rate analysis (Papoulis, 1991), the probability density function *f*(τ_{ab}) of the waiting time is:

We used an Arrhenius expression for the rate constant: α_{ab}(*t*) = α^{o}_{ab} exp{*q*_{ab}*x*_{ab}*V*(*t*)/*kT* }. *V*(*t*) is given by *V*_{o} + *mt*, where *V*_{o} is the ramp potential at time zero (i.e., the time at which the channel entered state *a*) and *m* is the ramp speed in units of voltage per unit time. The variable *q*_{ab} is the transition gating charge movement, and *x*_{ab} is the fractional position of the activation barrier between states *a* and *b*. By integrating the expression for conservation of probability, *f*(τ_{ab})dτ_{ab} = *f*(*r*_{n})d*r*_{n} (Papoulis, 1991), we obtain the following relationship between the random variables τ_{ab} and *r*_{n}:

In the event of competing transitions out of state *a* (multiple *b* states possible), selection was made by generating a waiting time for each one and choosing the smallest value. The single channel gating current record *i*_{g}(*t*) was constructed by binning transition impulses weighted by *q*_{ab} onto the discretized time axis. For the single channel ionic current record *i*(*t*), we used the formula *i* = *g*(*V* − *V*_{x}), where *g* is the conductance of the resident state, and *V*_{x} is the reversal potential of the permeant ion(s). The single channel traces were digitally filtered using a Gaussian filter with cutoff frequency *f*_{c}and delay 1/2*f*_{c} (which approximates a multipole Bessel filter; see Crouzy and Sigworth, 1993) and accumulated to produce macroscopic currents. To obtain a quantity proportional to the open probability, the mean ionic current was divided by the driving force, (*V* + 100) mV, for all ramp voltages *V*. Eq. 3 was used to obtain the sample estimate of the mean activation charge displacement, *q*^{_ }_{a}, except that the expression {d *P*_{o}/ d*V* }/*P*_{o} was evaluated instead of the equivalent d(ln*P*_{o})/d*V* in order to reduce round-off error. The ramp *Q* -*V* curve was obtained from the integral of the mean gating current. The software used in numerical calculations and the Monte Carlo simulation was written in the C programming language and was run on a 60 mHz Pentium processor.

## Results

We now demonstrate the theory with a series of numerical examples illustrated by Figs. 2–8. Starting with the simple discrete state models (Figs. 2–4), one or more schematic state diagrams are shown in increasing value of *q* on the left side of each figure. Following standard kinetic notation, allowable transitions between discrete states are indicated by a line labeled with the corresponding gating charge movement. This is done mainly because a kinetic model is more familiar looking than a random assortment of disconnected states, but it must be kept in mind that the nature and arrangement of connections between states are irrelevant for calculations of equilibrium quantities (such as *P*_{o} and 〈*q*_{a}〉), so long as a path exists which connects all states, and the time required for equilibration is much shorter than the length of the experiment. It is easy to see that the theoretical equations derived earlier are in accordance with this general rule, and they hold for models with continuous as well as discrete densities of states.

For all models we considered, whether discrete or continuous, we set the total essential charge movement Δ*q*_{e} equal to 4 eu to facilitate comparisons between models. Associated with each example are numerically derived plots of the equilibrium values of the gating charge displacement *Q* (normalized to one, as is normally done in practice) and the mean open probability *P*_{o} (actual value). The mean activation charge displacement 〈*q*_{a}〉 and the value of Δ*q* -〈*q*〉, also numerically derived, are featured in Fig. 2 *C*. Recall that the quantities *Q* and 〈*q*〉 are related by a factor of *N*, so they both have the same shape when normalized. Although we sometimes appear to use them interchangeably, we use *Q* when referring to experimental gating charge measurements where *N* is not known, whereas 〈*q*〉 is the mean of the single channel gating charge displacement, which is not directly measurable.

The discrete state models in Figs. 2–4 share the following features: the zero voltage potential *G*_{i}is the same for each state, though this is not explicitly shown in the figures. This tends to center the activation curves around *V* = 0. The closed states (*f* = 0) are labeled “C.” Similarly, “O” stands for open (*f* = 1).

### Two-state Model

Model 2*a* (Fig. 2) is a simple two state model, in which the total charge movement of 4 eu occurs in a single transition. A property of any two-state model is that all equilibrium properties lie on the same Boltzmann curve after normalization (Lumry et al., 1966). Thus the *P*_{o}-*V* and *Q* -*V* curves superimpose, and, because the two states are equipotential, the plots are centered around *V* = 0. Since there is only one open state and no peripheral charge movement, the model represents a saturated channel (see *Theory*). It is also the simplest example which satisfies Almers' criterion. Fig. 2 *B* shows the superposition of the plots of 〈*q*_{a}〉 and Δ*q* -〈*q*〉, which demonstrates graphically that the limiting value of 〈*q*_{a}〉 is reached only at potentials where the *Q* -*V* curve is close to saturating.

### Three-state Nonsequential Models

We relax the restriction to linear sequential models with models *b* and *c* of Fig. 2. In both cases we see a parallel movement of 4 eu that either converges to a single open state (model 2*b*) or diverges into two open states (model 2*c*). The total range of gating charge movement for each model is not 8 eu, but rather 4 eu, since state probability is split equally among the two pathways. As a rule, the maximal charge movement of a model containing communicating parallel paths is simply the largest net charge movement of any of the possible pathways. Both models 2*b* and 2*c* represent saturated channels. In the case of model 2*c*, although there are two open states, they are degenerate with respect to *q* (φ(open) = 2), producing no latent charge movement. The addition of an extra state merely shifts each Boltzmann plot to one side, without a change in the steepness of the curve at midpoint. This is because a state degeneracy produces an increase in entropy in the respective state. For example, in model 2*b*, setting *V* = 0 distributes 2/3 of the system probability to the two closed states, which lowers 〈*q*〉 and *P*_{o}. The same reasoning applied to other potentials explains why the equilibrium curves for model 2*b* are shifted to the right on the voltage axis. Similarly, the degenerate open state of model 2*c* produces a shift to the left.

As mentioned earlier, a different arrangement of allowable transitions in a particular model does not change the equilibrium values of state variables. For example, in model 2*c*, a line could be drawn between the two open states, and one of the existing lines from the closed state deleted, and the results shown in Fig. 2, *A* and *B*, would be unchanged. However, the kinetics of activation, which are not of concern here, but are an important determinant of channel function, would be drastically altered by such a change.

### Three-state Linear Sequential Models

In channels with three or more nondegenerate states, we do not expect activation curves representing different thermodynamic quantities to coincide. By inserting an extra closed state into the activation pathway of model 2*a*, we displace the *P*_{o}-*V* to the right of center and slightly broaden the *Q* -*V* (Fig. 3,*A*). However, this model remains saturated since it satisfies Almers' criterion of a linear sequence of closed states followed by one open state. Thus, 〈*q*_{a}〉 and Δ*q* -〈*q*〉 superimpose (Fig. 3 *B*), and the limiting slope procedure could be accurately used to measure total charge movement per channel.

Switching the positions of the open state and its neighboring closed state results in model 3*b*, which now has a closed state at the end of the activation pathway. The *Q* -*V* curve is unchanged but the *P*_{o}-*V* now approaches zero at positive as well as negative potentials. An example of this behavior may be seen in a channel experiencing voltage-dependent block (Bezanilla and Armstrong, 1972). Here we have the first example in which the open state appears in the middle of the activation sequence, and so we expect 〈*q*_{l}〉 to have a finite (but constant) value. Indeed, we see that the plot of 〈*q*_{a}〉 vs. *V* is displaced downward by a constant value of 2 eu (Fig. 3,*D*). Consequently, 〈*q*_{a}〉 becomes negative at depolarizing potentials, which comes about because the open probability decreases with increasing positive potential. Note that the total range of 〈*q*_{a}〉, which we will refer to as Δ〈*q*_{a}〉, is still 4 eu, though the limiting slope value in the hyperpolarizing direction (which we will refer to as Δ*q*_{a+}, see Figs. 1,*B* and 3 *D*) is only 2 eu and would by itself give an underestimate of Δ*q*. Thus, in order to correctly estimate the entire range of gating charge movement in this case, one would also need to apply the limiting slope procedure to depolarized potentials to obtain the negative component of the mean activation charge displacement (Δ*q*_{a−}). Model 3*b* remains an example of a saturated channel, since there is only one open state and no peripheral charge movement.

In the last model of Fig. 3 (model 3*c*), there are two open states in sequence at the end of activation. The *Q* -*V* curve is still unchanged, but now the *P*_{o}-*V* is shifted to the left of center. This is due to gating charge movement between open states, leading to a positive value for 〈*q*_{l}〉, which is now a function of voltage. This channel is not saturated. The range in mean activation charge displacement Δ〈*q*_{a}〉 reflects only the initial transition from the closed to the first open state. Hence the limiting slope procedure applied to this particular model underestimates Δ*q* by one half its value. In contrast, the *Q*/*N* procedure will give the correct value of Δ*q* for this model since it measures all essential charge movement. Although model 3*c* is displayed in Fig. 3 as a linear sequential model, the same outcome arises from a branching model in which a closed state makes transitions to two open states with respective gating charge movements, 2 eu and 4 eu (compare to model 2*c*, but with unequal charge movement per leg). Branching models, although useful in studying kinetics, are no different than linear sequential models in their equilibrium properties.

### Models with Peripheral Charge

In Fig. 4 we demonstrate the effects of charge movement energetically uncoupled to the main activation pathway (peripheral charge movement). Model 4*a* represents a saturated channel with a looped network of four closed states converging to an open state. The range in gating charge displacement Δ*q* is 4 eu and is entirely essential. By severing the links between the upper and lower charge relay systems, we obtain model 4*b*, which has two independent charge systems, with only the lower one linked to activation. If one were to measure the total range of 〈*q*〉 in this fragmented model, one would find it to be 6 eu, not 4 (if this is not immediately obvious, consider that we routinely sum the charge movements of *N* independent channels to obtain the gating current; also, the sum of all state probabilities in model 4*b* gives two, rather than one as in model 4*a*). The range in essential charge movement is unchanged (Δ*q*_{e} = 4 eu), but now, due to the additional peripheral charge movement Δ*q*_{p} of 2 eu, there is a mismatch between the limiting value of 〈*q*_{a}〉, which correctly estimates Δ*q*_{e}, and that of Δ*q* = *Δq*_{Q/N}, the value obtained if one were using the *Q*/*N* procedure. An example of peripheral charge movement present in neuronal α_{1E} Ca^{2+} channels has recently been demonstrated (Noceti et al., 1996) — in absence of the β_{2a} regulatory subunit, there appears to be a parallel charge system that, on the time scale of the observations, is kinetically isolated from the main activation sequence of the channel, leading to a *Δq*_{Q/N} value of 14 eu, but a value of only 9 eu for Δ*q*_{e}. With addition of the β_{2a} subunit to the system, the *Q*/*N* value dropped to the value of the limiting slope, which remained at 9 eu, suggesting that there was a lowering of the energy barrier which had separated the 5 eu of peripheral charge movement from the remainder, resulting in faster equilibration between the two charge systems. The β_{2a} subunit has no significant effect (<10 mV) on the half activation potential of the mean gating charge displacement or the initial rise of the open probability (Olcese et al., 1996), meaning that it is unlikely that the limiting slope value before addition of subunit was being selectively underestimated due to a larger voltage separation between the *Q* -*V* and the *P*_{o}-*V* plots.

### Models with Continuous Distribution of States

In Figs. 5–7, we shift our focus to continuous systems, where we will confirm some of the observations made above with discrete state systems, and encounter some new behavior. In these figures, the left side shows the potential profile *G*(*q*) as well as the fractional conductance *f*(*q*).

We begin with a flat free energy landscape for Fig. 5, which is implicitly the same assumption we have been making for all of the discrete state models described so far. The charge density is confined to within the boundaries *q* = 0 and *q* = Δ*q* = 4 eu. The function *f*(*q*) is zero (corresponding to closed states) for lower values of *q*, and then undergoes an abrupt change at *q* = *a*Δ*q* to a value of one (open state), where it remains until it reaches the upper boundary of *q*. Thus, this model has a varying amount of saturation which increases with the value of *a*. Of the discrete models we have considered so far, the most analogous to this model would be the model 3*c* of Fig. 3, since both are linear sequential (no degeneracies) with a finite amount of charge movement between open states. We concluded earlier in the discussion of Fig. 3 that the limiting value of 〈*q*_{a}〉 could never reach Δ*q* due to latent charge movement. This is shown to be the case as well with the continuum model, where it is apparent from Fig. 5,*B* that 〈*q*_{a}〉 reaches the maximum value of *a*Δ*q*. Note also the crossing of *P*_{o}-*V* with the normalized *Q* -*V* in Fig. 5 *A*, indicating the presence of multiple open states.

In Fig. 6 we demonstrate the effect of broadening *f*(*q*) around the gating charge position *q* = 0.9Δ*q*. We notice immediately a striking difference between the plots of 〈*q*_{a}〉 in Fig. 6 and those we have seen so far. The value of 〈*q*_{a}〉 plateaus without reaching the maximum value Δ*q,* and then appears to shrink to zero with increasing negative potential. The effect is more pronounced for broad distributions of *f*(*q*) than for very sharp ones. It would be quite interesting to see experimental evidence of the fall-off of 〈*q*_{a}〉 at negative potentials, since it would support the notion of subconductance states along the activation pathway. Incidently, a similar effect occurs in a discrete model similar to model 3*c*, if the last transition (between open states) moves significantly more charge than the first, leading to an early plateau in 〈*q*_{a}〉, which can be significantly larger in magnitude than the eventual limiting value seen at hyperpolarized potentials.

We choose for our final continuum model (Fig. 7) one which approximates a two-state model. Instead of a flat potential profile, we now introduce an inverted parabolic peak 4 *kT* high with a slight flattening at the edges and bounded on the *q*-axis at *q* = 0 and *q* = Δ*q* = 4. The channel is fully open for *q* values greater then 0.9 · Δ*q*. The result is a slightly broader equilibrium curve than for the true two state model (Fig. 2), and the *P*_{o}-*V* curve is a bit shifted to the right of the *Q* -*V*. However, the 〈*q*_{a}〉 and Δ*q*-〈*q*〉 plots coincide enough to make the difference in their limiting values (as could be obtained from limiting slope and *Q*/*N* methods, respectively) difficult to resolve experimentally, if this were a real channel.

### Multi-state Model with Subconductance States

Our concluding model (Fig. 8) shows that bizarre behavior of the equilibrium curves is not limited to continuum models. This model is discrete with five states. In contrast to the earlier discrete models we considered, we assign a different potential to each state, and we add subconductance states. Due to the small number of states, the plots of *P*_{o} and *Q* follow a somewhat erratic pathway. In a continuum model with a similar free energy landscape and the same approximate increase in *f*(*q*), the *P*_{o} vs. *V* and *Q*-*V* would broaden out and appear smoother. The voltage dependence of 〈*q*_{a}〉 shows some interesting behavior, increasing from zero at positive potentials to a local peak of about 1/4 Δ*q,* then dipping nearly to zero at more negative potentials, only to rise again to a maximum value slightly higher than that of the initial peak. Clearly, a plateau in the value of 〈*q*_{a}〉 may be misleading since it does not always represent the limiting slope value. The only way to be sure one has reached the final plateau is through comparison with the *Q*-*V*, which must be saturated in the range of potentials from which the limiting slope is recorded.

## Discussion

With the recent advances in molecular biology it has become possible to neutralize amino acids that are suspected to be voltage-sensing residues in ion channels and study the effects on gating. An important measure of channel responsiveness to voltage is the total charge movement of activation Δ*q*. A significant reduction of Δ*q* has been found after removal of charged residues in the S2 and S4 transmembrane domains of the *Shaker* potassium channel, indicating that these residues play an active role as components of the gating apparatus of the channel (Aggarwal and MacKinnon, 1996; Seoh et al., 1996). Almers (1978) summarized two methods by which one can obtain Δ*q* : (*a*) the *Q*/*N* procedure, which requires that one measure the maximum range of gating charge movement and the number of channels in the same preparation, and (*b*) the limiting value of the logarithmic potential sensitivity (similar to our mean activation charge displacement 〈*q*_{a}〉, except that *P*_{o}/[1 − *P*_{o}] replaces *P*_{o} as the argument of the logarithmic function), which equals the essential component of Δ*q* in the absence of latent charge movement.

Using a statistical mechanics approach, we have expanded on Almers' theory by explicitly expressing 〈*q*_{a}〉 = *kT*d(ln*P*_{o})/d*V* as a function of gating charge displacement, and by generalizing the result to include parallel activation pathways, multiple open states, subconductance states, and continuum models. The outcome of the derivation can be summarized by the following relation:

.

In cases where the ion channel is saturated and 〈*q*_{l}〉 is zero, Eq. 15 reduces to Almers' original expression for the limiting slope (Eq. 1) at hyperpolarizing potentials where the *Q* -*V* curve saturates (〈*q*〉 = 0).

A major obstacle in correctly estimating Δ*q* using the limiting slope method is the accurate determination of 〈*q*_{a}〉 at potentials where the open probability is vanishingly small. This problem has been discussed by several authors (Andersen and Koeppe, 1992; Bezanilla and Stefani, 1994; Zagotta et al., 1994), but no criterion has been given to accept or reject the estimate except to take the value as a lower limit of the actual Δ*q*. A useful guideline is provided by plotting 〈*q*_{a}〉 as a function of *V* or *P*_{o} (Zagotta et al., 1994) where it is possible to visualize whether the estimate shows signs of reaching a limiting value. Such limiting values have been observed in a few cases through single channel analysis in sodium channels (Hirschberg et al., 1996) or with macroscopic currents in neutralization mutants of *Shaker* K^{+} channels (Noceti et al. 1996; Seoh et al., 1996). Often, however, poor experimental resolution prohibits the measurement of a sufficiently low value of *P*_{o}, making a prediction of where the value of 〈*q*_{a}〉 saturates extremely useful. This is possible, based on Eq. (16), if the *Q-V* curve is known and the channel is saturated. What needs to be done is to invert the *Q* -*V* curve and scale it so that it superimposes onto the incomplete plot of 〈*q*_{a}〉 vs. *V*. It is important that a large enough range of voltage is used to insure good overlap between the two curves so that proper scaling is achieved. The value of Δ*q* is then read off from the scaled *Q* -*V* curve (Seoh et al., 1996).

An example of estimating Δ*q* with limited resolution data is shown in Fig. 9. The data was obtained from a Monte Carlo simulation of gating and ionic currents following a ramp voltage protocol (see methods). The model is shown in the lower right corner of Fig. 9 and has five closed states followed by an open state. All five transitions move an identical amount of gating charge for a total of Δ*q* = 10 eu. The ramp protocol is a useful experimental tool since it allows measurements of the signal for a large number of voltages in a single record. This is important when one is required to differentiate a measured quantity with respect to voltage, as we do when evaluating Eq. 3. The drawback in the method is that the ramp speed must be infinitely slow (quasi-static) for the channel to remain close to equilibrium during the ramp. Nevertheless, the alternative procedure of obtaining equilibrium values of ionic and gating currents from an activation series of pulses can be prohibitively difficult if one desires very fine resolution in voltage, making the ramp protocol the method of choice in certain cases (e.g., the presence of rundown in the preparation). In our simulation the midpoint of the integral of the mean gating current was shifted +2.5 mV with respect to the midpoint of the numerically derived *Q* -*V*, indicating that the quasistatic condition was not rigorously adhered to. This error will be evident in the final result. Fig. 9,*B* contains three plots. The estimate *q*^{– }_{a} and the ramp *Q* -*V* were calculated from the averaged ionic and gating currents plotted in Fig. 9 *A*. The numerical *Q* -*V* was derived from the model (experimentally, it can be accurately obtained from a voltage series of long pulses, Stefani et al., 1994). It is apparent that the scatter in *q*^{– }_{a} increases significantly with low *P*_{o} due to the increasing rarity of open events. The minimum value of *P*_{o} obtained in the plot of *q*^{– }_{a} was 5 × 10^{−3}, which is insufficient to reach the expected limiting value of 10 eu. Because the model satisfies Almers' criterion, we can use the inverted *Q* -*V* curves to “predict” the value of Δ*q* by scaling them so they superimpose onto the foot of the plot of *q*^{– }_{a} vs. *V*. We see that, due to the insufficiently slow ramp speed, the predictions from the ramp *Q* -*V* curve and true *Q* -*V* curve are both 10% in error, with the real value of Δ*q* lying approximately in between the two values. Thus, experimentally, it is important to use as slow a ramp speed as possible. This procedure was applied to the *Shaker* B K^{+} channel and charge neutralization mutants by Seoh et al. (1996). Their results show that for many of the mutations on the S2 and S4 putative transmembrane domains, the inverted and scaled *Q* -*V* curve superimposes on the *q*^{– }_{a} vs *V* curve. The predicted value of the limiting slope matched the value of Δ*q* obtained by the *Q*/*N* procedure, providing an internal check for consistency and at the same time showing that all charge that moves in *Shaker* is energetically coupled to the open state.

We conclude our discussion by suggesting an approach for measuring total gating charge movement in a generalized ion channel. A useful analysis should separate the gating charge into its components of peripheral, latent, and activation charge displacements. Latent charge movement comes about when gating charge moves during a transition between two or more discrete open or subconductance states, or along a continuum. Analysis of single channel records may uncover kinetically distinct discrete open states and/or subconductance states. Rate constants between successive open states may be voltage dependent, suggesting latent charge movement. Another useful test for the presence of latent charge movement in a channel that opens with depolarization is performed by comparing *P*_{o}-*V* and *Q* -*V* traces gathered from macroscopic currents. If the two plots cross, or if the *P*_{o} is shifted to the left of the *Q* -*V*, latent charge movement exists and the limiting slope procedure will underestimate the range of essential charge movement (e.g., Fig. 3,*F* ). Oftentimes, noise analysis of macroscopic ionic currents is easier to carry out than single channel analysis. In such cases, a nonparabolic variance vs. mean plot of nonstationary ionic currents (Steffan and Heinemann, 1996) points at the presence of subconductance states. Also, autocovariance analysis of stationary macroscopic ionic currents can detect multiple open states (Sigworth, 1981). If the channel has latent charge movement, it is not saturated with activation charge, and the range of activation charge Δ*q*_{a} is necessarily less than the range of essential charge movement Δ*q*_{e}. It must be kept in mind that the complete range in 〈*q*_{a}〉 spans from maximally negative to maximally positive potentials, and in cases where the channel closes with extreme potential on either side of the voltage axis, the limiting slope procedure must be carried out at positive as well as negative potentials (e.g., Fig. 3,*D*). In a saturated channel, the limiting slope procedure can be used to estimate Δ*q*_{e}, but lack of experimental resolution often makes it difficult to determine at which potential a limiting value of the activation charge displacement is reached. This is where the *Q* -*V* plot becomes invaluable, since the *Q* -*V* and the 〈*q*_{a}〉*-V* plots plateau at the same voltage range in saturated channels. The value of *Q* is easier to measure than 〈*q*_{a}〉 (assuming ionic currents can be effectively eliminated) near the region of limiting slope, since the relation of *Q* with gating charge displacement is linear, whereas that of 〈*q*_{a}〉 to *P*_{o} is obtained through differentiation, which amplifies the measurement error. Thus, the *Q* -*V* is a much more sensitive tool at determining the voltage at which 〈*q*_{a}〉 will saturate and can even be used to predict the value of Δ*q*_{e} from low-resolution data (Fig. 9). There may be instances when a *Q* -*V* is unobtainable (inadequate expression of channels, incomplete blocking of the pore, etc.). In such cases, an alternate method (Cole-Moore shift) for determining whether 〈*q*_{a}〉 has reached its final value may prove useful as a last resort. The Cole-Moore shift is defined as the time delay of opening of the channel as a function of holding potential (Cole and Moore, 1960; Stefani et al., 1994)). At those potentials where 〈*q*_{a}〉 has reached saturation, the delay should also have reached its maximum value. It should be kept in mind, however, that the Cole-Moore shift is a kinetic measurement, even though its voltage dependence arises from the equilibrium probability distribution at the holding potential. Thus, unlike the *Q* -*V*, the plot of opening delay vs. voltage has no functional relationship with 〈*q*_{a}〉 vs. voltage. Nevertheless, the initial probability distribution does not change beyond the voltage at which the gating charge saturates, so in principle the Cole-Moore shift, if accurately measured, could serve as a poor man's *Q* -*V* in limiting slope experiments.

A separate issue is whether or not there is contamination of the gating charge movement with a peripheral (independent) charge system. Peripheral charge movement shows up in the *Q*/*N* estimate of total gating charge movement, so Δ*q*_{Q/N} will be larger than Δ*q*_{e} in the presence of peripheral charge. Combining this result and the earlier one, which set the upper limit of Δ*q*a as Δ*q*_{e}, we obtain the inequality:

If the values of Δ*q* a and *Δq*_{Q/N} are the same, it is a good indicator that there is neither latent nor peripheral charge movement, and the estimate of Δ*q*_{e} is an accurate one. If both latent and peripheral charge are associated with the same channel, it may be difficult to determine the contribution of each. In such a case, kinetic modeling might be required in order to estimate the amount of charge movement between open states through the voltage dependence of the transition rate constants.

In summary, when measuring Δ*q*_{e}, the range in essential charge movement in a single channel, it is desirable to obtain the full activation curves of the open probability and gating charge displacement. For channels without latent charge movement, the limiting slope procedure, in conjunction with information from the *Q-V* plot, will produce an accurate estimate of Δ*q*_{e}. In the general case, the value of Δ*q*_{e} will lie between the range of activation charge displacement, Δ*q*_{a}, and the total charge movement per channel, *Δq*_{Q/N}, obtained from the limiting slope method and *Q*/*N* procedure, respectively.

## Acknowledgments

We thank Drs. Dorine Starace, David E. Patton, Francesca Noceti, and Enrico Stefani for reading and commenting on the manuscript.

This work was supported by United States Public Health Service grant GM30376 and a Dissertation Fellowship from the Graduate Division at UCLA to D. Sigg.

## Abbreviation used in this paper

## references

## Author notes

Address correspondence to Dr. F. Bezanilla or D. Sigg, Department of Physiology, UCLA School of Medicine, Los Angeles, CA 90095. FAX: 310-794-9612; E-mail: pancho@cvmail.anes.ucla.edu